Physics Formulary - J. Wevers

Physics Formulary

By ir. J.C.A. Wevers

Contents Contents

I

Physical Constants

1

1 Mechanics 1.1 Point-kinetics in a fixed coordinate system . . . . . . . . 1.1.1 Definitions . . . . . . . . . . . . . . . . . . . . 1.1.2 Polar coordinates . . . . . . . . . . . . . . . . . 1.2 Relative motion . . . . . . . . . . . . . . . . . . . . . . 1.3 Point-dynamics in a fixed coordinate system . . . . . . . 1.3.1 Force, (angular)momentum and energy . . . . . 1.3.2 Conservative force fields . . . . . . . . . . . . . 1.3.3 Gravitation . . . . . . . . . . . . . . . . . . . . 1.3.4 Orbital equations . . . . . . . . . . . . . . . . . 1.3.5 The virial theorem . . . . . . . . . . . . . . . . 1.4 Point dynamics in a moving coordinate system . . . . . 1.4.1 Apparent forces . . . . . . . . . . . . . . . . . . 1.4.2 Tensor notation . . . . . . . . . . . . . . . . . . 1.5 Dynamics of masspoint collections . . . . . . . . . . . . 1.5.1 The centre of mass . . . . . . . . . . . . . . . . 1.5.2 Collisions . . . . . . . . . . . . . . . . . . . . . 1.6 Dynamics of rigid bodies . . . . . . . . . . . . . . . . . 1.6.1 Moment of Inertia . . . . . . . . . . . . . . . . 1.6.2 Principal axes . . . . . . . . . . . . . . . . . . . 1.6.3 Time dependence . . . . . . . . . . . . . . . . . 1.7 Variational Calculus, Hamilton and Lagrange mechanics 1.7.1 Variational Calculus . . . . . . . . . . . . . . . 1.7.2 Hamilton mechanics . . . . . . . . . . . . . . . 1.7.3 Motion around an equilibrium, linearization . . . 1.7.4 Phase space, Liouville’s equation . . . . . . . . 1.7.5 Generating functions . . . . . . . . . . . . . . .

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2 2 2 2 2 2 2 3 3 3 4 4 4 5 5 5 5 6 6 6 6 6 6 7 7 7 8

2 Electricity & Magnetism 2.1 The Maxwell equations . . . . . . . . . . 2.2 Force and potential . . . . . . . . . . . . 2.3 Gauge transformations . . . . . . . . . . 2.4 Energy of the electromagnetic field . . . . 2.5 Electromagnetic waves . . . . . . . . . . 2.5.1 Electromagnetic waves in vacuum 2.5.2 Electromagnetic waves in matter . 2.6 Multipoles . . . . . . . . . . . . . . . . . 2.7 Electric currents . . . . . . . . . . . . . . 2.8 Depolarizing field . . . . . . . . . . . . . 2.9 Mixtures of materials . . . . . . . . . . .

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Physics Formulary by ir. J.C.A. Wevers

II

3 Relativity 3.1 Special relativity . . . . . . . . . . . . . . . . . . 3.1.1 The Lorentz transformation . . . . . . . . 3.1.2 Red and blue shift . . . . . . . . . . . . . 3.1.3 The stress-energy tensor and the field tensor 3.2 General relativity . . . . . . . . . . . . . . . . . . 3.2.1 Riemannian geometry, the Einstein tensor . 3.2.2 The line element . . . . . . . . . . . . . . 3.2.3 Planetary orbits and the perihelion shift . . 3.2.4 The trajectory of a photon . . . . . . . . . 3.2.5 Gravitational waves . . . . . . . . . . . . . 3.2.6 Cosmology . . . . . . . . . . . . . . . . .

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13 13 13 14 14 14 14 15 16 17 17 17

4 Oscillations 4.1 Harmonic oscillations . . . . . . . . . 4.2 Mechanic oscillations . . . . . . . . . 4.3 Electric oscillations . . . . . . . . . . 4.4 Waves in long conductors . . . . . . . 4.5 Coupled conductors and transformers 4.6 Pendulums . . . . . . . . . . . . . . .

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5 Waves 5.1 The wave equation . . . . . . . . . . . . . . 5.2 Solutions of the wave equation . . . . . . . . 5.2.1 Plane waves . . . . . . . . . . . . . . 5.2.2 Spherical waves . . . . . . . . . . . . 5.2.3 Cylindrical waves . . . . . . . . . . . 5.2.4 The general solution in one dimension 5.3 The stationary phase method . . . . . . . . . 5.4 Green functions for the initial-value problem . 5.5 Waveguides and resonating cavities . . . . . 5.6 Non-linear wave equations . . . . . . . . . .

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6 Optics 6.1 The bending of light . . . . . . 6.2 Paraxial geometrical optics . . 6.2.1 Lenses . . . . . . . . 6.2.2 Mirrors . . . . . . . . 6.2.3 Principal planes . . . . 6.2.4 Magnification . . . . . 6.3 Matrix methods . . . . . . . . 6.4 Aberrations . . . . . . . . . . 6.5 Reflection and transmission . . 6.6 Polarization . . . . . . . . . . 6.7 Prisms and dispersion . . . . . 6.8 Diffraction . . . . . . . . . . . 6.9 Special optical effects . . . . . 6.10 The Fabry-Perot interferometer

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7 Statistical physics 7.1 Degrees of freedom . . . . . . . 7.2 The energy distribution function 7.3 Pressure on a wall . . . . . . . . 7.4 The equation of state . . . . . . 7.5 Collisions between molecules . .

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Physics Formulary by ir. J.C.A. Wevers

7.6

III

Interaction between molecules . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . .

8 Thermodynamics 8.1 Mathematical introduction . . . . . . 8.2 Definitions . . . . . . . . . . . . . . . 8.3 Thermal heat capacity . . . . . . . . . 8.4 The laws of thermodynamics . . . . . 8.5 State functions and Maxwell relations 8.6 Processes . . . . . . . . . . . . . . . 8.7 Maximal work . . . . . . . . . . . . . 8.8 Phase transitions . . . . . . . . . . . 8.9 Thermodynamic potential . . . . . . . 8.10 Ideal mixtures . . . . . . . . . . . . . 8.11 Conditions for equilibrium . . . . . . 8.12 Statistical basis for thermodynamics . 8.13 Application to other systems . . . . .

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9 Transport phenomena 9.1 Mathematical introduction . . . . . . . . . . . . . 9.2 Conservation laws . . . . . . . . . . . . . . . . . . 9.3 Bernoulli’s equations . . . . . . . . . . . . . . . . 9.4 Characterising of flows by dimensionless numbers . 9.5 Tube flows . . . . . . . . . . . . . . . . . . . . . . 9.6 Potential theory . . . . . . . . . . . . . . . . . . . 9.7 Boundary layers . . . . . . . . . . . . . . . . . . . 9.7.1 Flow boundary layers . . . . . . . . . . . . 9.7.2 Temperature boundary layers . . . . . . . . 9.8 Heat conductance . . . . . . . . . . . . . . . . . . 9.9 Turbulence . . . . . . . . . . . . . . . . . . . . . 9.10 Self organization . . . . . . . . . . . . . . . . . .

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10 Quantum physics 10.1 Introduction to quantum physics . . . . . . . 10.1.1 Black body radiation . . . . . . . . . . 10.1.2 The Compton effect . . . . . . . . . . 10.1.3 Electron diffraction . . . . . . . . . . . 10.2 Wave functions . . . . . . . . . . . . . . . . . 10.3 Operators in quantum physics . . . . . . . . . 10.4 The uncertainty principle . . . . . . . . . . . 10.5 The Schr¨odinger equation . . . . . . . . . . . 10.6 Parity . . . . . . . . . . . . . . . . . . . . . . 10.7 The tunnel effect . . . . . . . . . . . . . . . . 10.8 The harmonic oscillator . . . . . . . . . . . . 10.9 Angular momentum . . . . . . . . . . . . . . 10.10 Spin . . . . . . . . . . . . . . . . . . . . . . 10.11 The Dirac formalism . . . . . . . . . . . . . . 10.12 Atomic physics . . . . . . . . . . . . . . . . 10.12.1 Solutions . . . . . . . . . . . . . . . 10.12.2 Eigenvalue equations . . . . . . . . . 10.12.3 Spin-orbit interaction . . . . . . . . . 10.12.4 Selection rules . . . . . . . . . . . . . 10.13 Interaction with electromagnetic fields . . . . 10.14 Perturbation theory . . . . . . . . . . . . . . 10.14.1 Time-independent perturbation theory 10.14.2 Time-dependent perturbation theory .

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Physics Formulary by ir. J.C.A. Wevers

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10.15 N-particle systems 10.15.1 General . 10.15.2 Molecules 10.16 Quantum statistics

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11 Plasma physics 11.1 Introduction . . . . . . . . . . . . . . . . . . 11.2 Transport . . . . . . . . . . . . . . . . . . . 11.3 Elastic collisions . . . . . . . . . . . . . . . 11.3.1 General . . . . . . . . . . . . . . . . 11.3.2 The Coulomb interaction . . . . . . . 11.3.3 The induced dipole interaction . . . . 11.3.4 The centre of mass system . . . . . . 11.3.5 Scattering of light . . . . . . . . . . . 11.4 Thermodynamic equilibrium and reversibility 11.5 Inelastic collisions . . . . . . . . . . . . . . 11.5.1 Types of collisions . . . . . . . . . . 11.5.2 Cross sections . . . . . . . . . . . . 11.6 Radiation . . . . . . . . . . . . . . . . . . . 11.7 The Boltzmann transport equation . . . . . . 11.8 Collision-radiative models . . . . . . . . . . 11.9 Waves in plasma’s . . . . . . . . . . . . . . .

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62 62 62 63 63 63 63 64 65 65 65 65 66 66 66 67 67 67 67 68 68 69 69 70 70 70

12 Solid state physics 12.1 Crystal structure . . . . . . . . . . . . . . . . . . . 12.2 Crystal binding . . . . . . . . . . . . . . . . . . . 12.3 Crystal vibrations . . . . . . . . . . . . . . . . . . 12.3.1 A lattice with one type of atoms . . . . . . 12.3.2 A lattice with two types of atoms . . . . . 12.3.3 Phonons . . . . . . . . . . . . . . . . . . . 12.3.4 Thermal heat capacity . . . . . . . . . . . 12.4 Magnetic field in the solid state . . . . . . . . . . . 12.4.1 Dielectrics . . . . . . . . . . . . . . . . . 12.4.2 Paramagnetism . . . . . . . . . . . . . . . 12.4.3 Ferromagnetism . . . . . . . . . . . . . . 12.5 Free electron Fermi gas . . . . . . . . . . . . . . . 12.5.1 Thermal heat capacity . . . . . . . . . . . 12.5.2 Electric conductance . . . . . . . . . . . . 12.5.3 The Hall-effect . . . . . . . . . . . . . . . 12.5.4 Thermal heat conductivity . . . . . . . . . 12.6 Energy bands . . . . . . . . . . . . . . . . . . . . 12.7 Semiconductors . . . . . . . . . . . . . . . . . . . 12.8 Superconductivity . . . . . . . . . . . . . . . . . . 12.8.1 Description . . . . . . . . . . . . . . . . . 12.8.2 The Josephson effect . . . . . . . . . . . . 12.8.3 Flux quantisation in a superconducting ring 12.8.4 Macroscopic quantum interference . . . . . 12.8.5 The London equation . . . . . . . . . . . . 12.8.6 The BCS model . . . . . . . . . . . . . . .

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Physics Formulary by ir. J.C.A. Wevers

V

13 Theory of groups 13.1 Introduction . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . 13.1.1 Definition of a group . . . . . . . . . . . . . . . . . . . . . . . . . . 13.1.2 The Cayley table . . . . . . . . . . . . . . . . . . . . . . . . . . . . 13.1.3 Conjugated elements, subgroups and classes . . . . . . . . . . . . . . 13.1.4 Isomorfism and homomorfism; representations . . . . . . . . . . . . 13.1.5 Reducible and irreducible representations . . . . . . . . . . . . . . . 13.2 The fundamental orthogonality theorem . . . . . . . . . . . . . . . . . . . . 13.2.1 Schur’s lemma . . . . . . . . . . . . . . . . . . . . . . . . . . . . . 13.2.2 The fundamental orthogonality theorem . . . . . . . . . . . . . . . . 13.2.3 Character . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . 13.3 The relation with quantum mechanics . . . . . . . . . . . . . . . . . . . . . 13.3.1 Representations, energy levels and degeneracy . . . . . . . . . . . . 13.3.2 Breaking of degeneracy by a perturbation . . . . . . . . . . . . . . . 13.3.3 The construction of a base function . . . . . . . . . . . . . . . . . . 13.3.4 The direct product of representations . . . . . . . . . . . . . . . . . 13.3.5 Clebsch-Gordan coefficients . . . . . . . . . . . . . . . . . . . . . . 13.3.6 Symmetric transformations of operators, irreducible tensor operators . 13.3.7 The Wigner-Eckart theorem . . . . . . . . . . . . . . . . . . . . . . 13.4 Continuous groups . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . 13.4.1 The 3-dimensional translation group . . . . . . . . . . . . . . . . . . 13.4.2 The 3-dimensional rotation group . . . . . . . . . . . . . . . . . . . 13.4.3 Properties of continuous groups . . . . . . . . . . . . . . . . . . . . 13.5 The group SO(3) . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . 13.6 Applications to quantum mechanics . . . . . . . . . . . . . . . . . . . . . . 13.6.1 Vectormodel for the addition of angular momentum . . . . . . . . . . 13.6.2 Irreducible tensor operators, matrixelements and selection rules . . . 13.7 Applications to particle physics . . . . . . . . . . . . . . . . . . . . . . . . .

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71 71 71 71 71 72 72 72 72 72 72 73 73 73 73 74 74 74 75 75 75 75 76 77 77 77 78 79

14 Nuclear physics 14.1 Nuclear forces . . . . . . . . . . . . . . . . . . . . . . . . . . . . . 14.2 The shape of the nucleus . . . . . . . . . . . . . . . . . . . . . . . 14.3 Radioactive decay . . . . . . . . . . . . . . . . . . . . . . . . . . . 14.4 Scattering and nuclear reactions . . . . . . . . . . . . . . . . . . . 14.4.1 Kinetic model . . . . . . . . . . . . . . . . . . . . . . . . . 14.4.2 Quantum mechanical model for n-p scattering . . . . . . . . 14.4.3 Conservation of energy and momentum in nuclear reactions 14.5 Radiation dosimetry . . . . . . . . . . . . . . . . . . . . . . . . . .

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81 81 82 82 83 83 83 84 84

15 Quantum field theory & Particle physics 15.1 Creation and annihilation operators . . . . . . . . . . . . . . . 15.2 Classical and quantum fields . . . . . . . . . . . . . . . . . . 15.3 The interaction picture . . . . . . . . . . . . . . . . . . . . . . 15.4 Real scalar field in the interaction picture . . . . . . . . . . . . 15.5 Charged spin-0 particles, conservation of charge . . . . . . . . 15.6 Field functions for spin- 21 particles . . . . . . . . . . . . . . . 15.7 Quantization of spin- 21 fields . . . . . . . . . . . . . . . . . . 15.8 Quantization of the electromagnetic field . . . . . . . . . . . . 15.9 Interacting fields and the S-matrix . . . . . . . . . . . . . . . . 15.10 Divergences and renormalization . . . . . . . . . . . . . . . . 15.11 Classification of elementary particles . . . . . . . . . . . . . . 15.12 P and CP-violation . . . . . . . . . . . . . . . . . . . . . . . . 15.13 The standard model . . . . . . . . . . . . . . . . . . . . . . . 15.13.1 The electroweak theory . . . . . . . . . . . . . . . . . 15.13.2 Spontaneous symmetry breaking: the Higgs mechanism

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85 85 85 86 86 87 87 88 89 89 90 90 92 93 93 94

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Physics Formulary by ir. J.C.A. Wevers

VI

15.13.3 Quantumchromodynamics . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . 15.14 Path integrals . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . 15.15 Unification and quantum gravity . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . 16 Astrophysics 16.1 Determination of distances . . . . 16.2 Brightness and magnitudes . . . . 16.3 Radiation and stellar atmospheres 16.4 Composition and evolution of stars 16.5 Energy production in stars . . . . The ∇-operator The SI units

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94 95 95 96 96 96 97 97 98 99 100

Physical Constants Name Number π Number e Euler’s constant

Symbol Value Unit π 3.14159265358979323846 e 2.71828182845904523536   n P γ = lim 1/k − ln(n) = 0.5772156649 n→∞

k=1

Elementary charge Gravitational constant Fine-structure constant Speed of light in vacuum Permittivity of the vacuum Permeability of the vacuum (4πε0 )−1

e G, κ α = e2 /2hcε0 c ε0 µ0

1.60217733 · 10−19 6.67259 · 10−11 ≈ 1/137 2.99792458 · 108 8.854187 · 10−12 4π · 10−7 8.9876 · 109

C m3 kg−1 s−2

Planck’s constant Dirac’s constant Bohr magneton Bohr radius Rydberg’s constant Electron Compton wavelength Proton Compton wavelength Reduced mass of the H-atom

h h = h/2π ¯ µB = e¯h/2me a0 Ry λCe = h/me c λCp = h/mp c µH

6.6260755 · 10−34 1.0545727 · 10−34 9.2741 · 10−24 0.52918 13.595 2.2463 · 10−12 1.3214 · 10−15 9.1045755 · 10−31

Js Js Am2 ˚ A eV m m kg

Stefan-Boltzmann’s constant Wien’s constant Molar gasconstant Avogadro’s constant Boltzmann’s constant

σ kW R NA k = R/NA

5.67032 · 10−8 2.8978 · 10−3 8.31441 6.0221367 · 1023 1.380658 · 10−23

Wm−2 K−4 mK J/mol mol−1 J/K

Electron mass Proton mass Neutron mass Elementary mass unit Nuclear magneton

me mp mn mu = µN

9.1093897 · 10−31 1.6726231 · 10−27 1.674954 · 10−27 1.6605656 · 10−27 5.0508 · 10−27

kg kg kg kg J/T

Diameter of the Sun Mass of the Sun Rotational period of the Sun Radius of Earth Mass of Earth Rotational period of Earth Earth orbital period Astronomical unit Light year Parsec Hubble constant

D M T RA MA TA Tropical year AU lj pc H

1392 · 106 1.989 · 1030 25.38 6.378 · 106 5.976 · 1024 23.96 365.24219879 1.4959787066 · 1011 9.4605 · 1015 3.0857 · 1016 ≈ (75 ± 25)

m kg days m kg hours days m m m km·s−1 ·Mpc−1

1 12 12 m( 6 C)

1

m/s (def) F/m H/m Nm2 C−2

Chapter 1

Mechanics 1.1 Point-kinetics in a fixed coordinate system 1.1.1 Definitions The position ~r, the velocity ~v and the acceleration ~a are defined by: ~r = (x, y, z), ~v = (x, ˙ y, ˙ z), ˙ ~a = (¨ x, y¨, z¨). The following holds: Z Z Z s(t) = s0 + |~v (t)|dt ; ~r(t) = ~r0 + ~v (t)dt ; ~v (t) = ~v0 + ~a(t)dt When the acceleration is constant this gives: v(t) = v0 + at and s(t) = s0 + v0 t + 12 at2 . For the unit vectors in a direction ⊥ to the orbit ~et and parallel to it ~en holds: ~et =

d~r ˙ ~v v ~e˙t = ~et = ~en ; ~en = |~v | ds ρ |~e˙t |

For the curvature k and the radius of curvature ρ holds: 2 ~k = d~et = d ~r = dϕ ; ρ = 1 ds ds ds2 |k|

1.1.2 Polar coordinates Polar coordinates are defined by: x = r cos(θ), y = r sin(θ). So, for the unit coordinate vectors holds: ˙eθ , ~e˙θ = −θ~ ˙ er ~e˙r = θ~ ˙eθ , ~a = (¨ ¨ eθ . The velocity and the acceleration are derived from: ~r = r~er , ~v = r~ ˙ er + rθ~ r − rθ˙2 )~er + (2r˙ θ˙ + rθ)~

1.2 Relative motion For the motion of a point D w.r.t. a point Q holds: ~rD = ~rQ +

~ω × ~vQ ˙ ~ = ~rD − ~rQ and ω = θ. with QD ω2

¨ 0 means that the quantity is defined in a moving system of coordinates. In a moving Further holds: α = θ. system holds: ω × ~r 0 and ~a = ~aQ + ~a 0 + α ~ × ~r 0 + 2~ω × ~v − ~ω × (~ω × ~r 0 ) ~v = ~vQ + ~v 0 + ~ 0 2 0 with |~ω × (~ ω × ~r )| = ω ~r n

1.3 Point-dynamics in a fixed coordinate system 1.3.1 Force, (angular)momentum and energy Newton’s 2nd law connects the force on an object and the resulting acceleration of the object where the momentum is given by p~ = m~v : d(m~v ) d~v dm m=const d~ p = =m + ~v = m~a F~ (~r, ~v , t) = dt dt dt dt 2

Chapter 1: Mechanics

3

Newton’s 3rd law is given by: F~action = −F~reaction . ˙ = F~ · ~v . For the total energy W , the kinetic energy T and the potential energy For the power P holds: P = W U holds: W = T + U ; T˙ = −U˙ with T = 12 mv 2 . Z ~ is given by: S ~ = ∆~ The kick S p = F~ dt Z2

Z2 F~ · d~s =

The work A, delivered by a force, is A = 1

F cos(α)ds 1

~ ~τ = L ~˙ = ~r × F~ ; and The torque ~τ is related to the angular momentum L: ~ = ~r × p~ = m~v × ~r, |L| ~ = mr2 ω. The following equation is valid: L ∂U ∂θ P P~ Fi = 0 and ~τi = 0. Hence, the conditions for a mechanical equilibrium are: τ =−

The force of friction is usually proportional to the force perpendicular to the surface, except when the motion starts, when a threshold has to be overcome: Ffric = f · Fnorm · ~et .

1.3.2 Conservative force fields ~ . From this follows that A conservative force can be written as the gradient of a potential: F~cons = −∇U ~ ~ ∇ × F = 0. For such a force field also holds: Zr1

I

F~ · d~s

F~ · d~s = 0 ⇒ U = U0 − r0

So the work delivered by a conservative force field depends not on the trajectory covered but only on the starting and ending points of the motion.

1.3.3 Gravitation The Newtonian law of gravitation is (in GRT one also uses κ instead of G): m1 m2 F~g = −G 2 ~er r The gravitational potential is then given by V = −Gm/r. From Gauss law it then follows: ∇2 V = 4πG%.

1.3.4 Orbital equations If V = V (r) one can derive from the equations of Lagrange for φ the conservation of angular momentum: ∂V d ∂L = = 0 ⇒ (mr2 φ) = 0 ⇒ Lz = mr2 φ = constant ∂φ ∂φ dt For the radial position as a function of time can be found that:  2 L2 2(W − V ) dr − 2 2 = dt m m r The angular equation is then: #−1 Zr " 2 r L2 2(W − V ) mr − 2 2 dr φ − φ0 = L m m r 0

r −2 field

=

arccos 1 +

1 r 1 r0

−

1 r0

!

+ km/L2z

If F = F (r): L =constant, if F is conservative: W =constant, if F~ ⊥ ~v then ∆T = 0 and U = 0.

Physics Formulary by ir. J.C.A. Wevers

4

Kepler’s orbital equations In a force field F = kr−2 , the orbits are conic sections with the origin of the force in one of the foci (Kepler’s 1st law). The equation of the orbit is: r(θ) =

` , or: x2 + y 2 = (` − εx)2 1 + ε cos(θ − θ0 )

with

` 2W L2 ` k L2 ; ε2 = 1 + 2 3 2 = 1 − ; a = = 2 2 Gµ Mtot G µ Mtot a 1−ε 2W a is half the√ length of the long axis of the elliptical orbit in case the orbit is closed. Half the length of the short axis is b = a`. ε is the excentricity of the orbit. Orbits with an equal ε are of equal shape. Now, 5 types of orbits are possible: `=

1. k < 0 and ε = 0: a circle. 2. k < 0 and 0 < ε < 1: an ellipse. 3. k < 0 and ε = 1: a parabole. 4. k < 0 and ε > 1: a hyperbole, curved towards the centre of force. 5. k > 0 and ε > 1: a hyperbole, curved away from the centre of force. Other combinations are not possible: the total energy in a repulsive force field is always positive so ε > 1. If the surface between the orbit covered between t1 and t2 and the focus C around which the planet moves is A(t1 , t2 ), Kepler’s 2nd law is LC (t2 − t1 ) A(t1 , t2 ) = 2m Kepler’s 3rd law is, with T the period and Mtot the total mass of the system: 4π 2 T2 = 3 a GMtot

1.3.5 The virial theorem The virial theorem for one particle is: D E hm~v · ~ri = 0 ⇒ hT i = − 12 F~ · ~r =

1 2

  k dU = 12 n hU i if U = − n r dr r

The virial theorem for a collection of particles is: * + X X F~i · ~ri + F~ij · ~rij hT i = − 12 particles

pairs

These propositions can also be written as: 2Ekin + Epot = 0.

1.4 Point dynamics in a moving coordinate system 1.4.1 Apparent forces The total force in a moving coordinate system can be found by subtracting the apparent forces from the forces working in the reference frame: F~ 0 = F~ − F~app . The different apparent forces are given by: 1. Transformation of the origin: For = −m~aa 2. Rotation: F~α = −m~ α × ~r 0 3. Coriolis force: Fcor = −2m~ω × ~v 2

mv ~er 4. Centrifugal force: F~cf = mω 2~rn 0 = −F~cp ; F~cp = − r

Chapter 1: Mechanics

5

1.4.2 Tensor notation Transformation of the Newtonian equations of motion to xα = xα (x) gives: ∂xα d¯ xβ dxα = ; β dt ∂x ¯ dt The chain rule gives: d2 xα d d dxα = = 2 dt dt dt dt so:

This leads to:



∂xα d¯ xβ ∂x ¯β dt



d¯ xβ d ¯β ∂xα d2 x + = ∂x ¯β dt2 dt dt



∂xα ∂x ¯β



∂ 2 xα d¯ ∂ ∂xα d¯ xγ xγ d ∂xα = = β γ β β γ dt ∂ x ¯ ∂x ¯ ∂x ¯ dt ∂x ¯ ∂x ¯ dt ∂xα d2 x¯β ∂ 2 xα d¯ xγ d2 xα = + dt2 ∂x ¯β dt2 ∂x ¯β ∂ x ¯γ dt



d¯ xβ dt



Hence the Newtonian equation of motion m will be transformed into:

 m

d2 xα = Fα dt2

d2 xα dxβ dxγ + Γα βγ 2 dt dt dt

 = Fα

The apparent forces are taken from he origin to the effect side in the way Γα βγ

dxβ dxγ . dt dt

1.5 Dynamics of masspoint collections 1.5.1 The centre of mass ~ is given by ~v − R. ~˙ The coordinates of the centre of mass are given by: The velocity w.r.t. the centre of mass R P mi~ri ~rm = P mi In a 2-particle system, the coordinates of the centre of mass are given by: ~ = m1~r1 + m2~r2 R m1 + m2 With ~r = ~r1 − ~r2 , the kinetic energy becomes: T = 12 Mtot R˙ 2 + 12 µr˙ 2 , with the reduced mass µ given by: 1 1 1 = + µ m1 m2 The motion within and outside the centre of mass can be separated: ~˙ inside = ~τinside ~˙ outside = ~τoutside ; L L p~ = m~vm ; F~ext = m~am ; F~12 = µ~u

1.5.2 Collisions With collisions, where B are the coordinates of the collision and C an arbitrary other position, holds: ~p = m~vm ~ = ∆~ is constant, and T = 12 m~vm2 is constant. The changes in the relative velocities can be derived from: S p= ~ C = CB ~ × S, ~ p~ k S ~ =constant and L ~ w.r.t. B is constant. µ(~vaft − ~vbefore ). Further holds ∆L

Physics Formulary by ir. J.C.A. Wevers

6

1.6 Dynamics of rigid bodies 1.6.1 Moment of Inertia The angular momentum in a moving coordinate system is given by: ~0 ~ 0 = I~ ω+L L n where I is the moment of inertia with respect to a central axis, which is given by: X mi~ri 2 ; T 0 = Wrot = 12 ωIij ~ei~ej = 12 Iω 2 I= i

or, in the continuous case: I=

m V

Z

r0 n dV = 2

Z

r0 n dm 2

Further holds: Li = I ij ωj ; Iii = Ii ; Iij = Iji = −

X

mk x0i x0j

k

Steiner’s theorem is: Iw.r.t.D = Iw.r.t.C + m(DM )2 if axis C k axis D. Object

I

Object

I

Cavern cylinder

I = mR2

Massive cylinder

I = 12 mR2

Disc, axis in plane disc through m

I = 14 mR2

Halter

I = 12 µR2

Cavern sphere

I = 23 mR2

Massive sphere

I = 25 mR2

Bar, axis ⊥ through c.o.m.

I=

1 2 12 ml

Bar, axis ⊥ through end

I = 13 ml2

Rectangle, axis ⊥ plane thr. c.o.m.

I=

1 2 12 m(a

Rectangle, axis k b thr. m

I = ma2

+ b2 )

1.6.2 Principal axes Each rigid body has (at least) 3 principal axes which stand ⊥ to each other. For a principal axis holds: ∂I ∂I ∂I = = = 0 so L0n = 0 ∂ωx ∂ωy ∂ωz The following holds: ω˙ k = −aijk ωi ωj with aijk =

Ii − Ij if I1 ≤ I2 ≤ I3 . Ik

1.6.3 Time dependence For torque of force ~τ holds: ~τ 0 = I θ¨ ;

~0 d00 L ~0 = ~τ 0 − ~ω × L dt

~ The torque T~ is defined by: T~ = F~ × d.

1.7 Variational Calculus, Hamilton and Lagrange mechanics 1.7.1 Variational Calculus Starting with:



Zb L(q, q, ˙ t)dt = 0 with δ(a) = δ(b) = 0 and δ

δ a

du dx

 =

d (δu) dx

Chapter 1: Mechanics

7

the equations of Lagrange can be derived: ∂L d ∂L = dt ∂ q˙i ∂qi When there are additional conditions applying to the variational problem δJ(u) = 0 of the type K(u) =constant, the new problem becomes: δJ(u) − λδK(u) = 0.

1.7.2 Hamilton mechanics P P The Lagrangian is given by: L = T (q˙i ) − V (qi ). The Hamiltonian is given by: H = q˙i pi − L. In 2 dimensions holds: L = T − U = 12 m(r˙ 2 + r2 φ˙ 2 ) − U (r, φ). If the used coordinates are canonical the Hamilton equations are the equations of motion for the system: ∂H dqi = ; dt ∂pi

∂H dpi =− dt ∂qi

Coordinates are canonical if the following holds: {qi , qj } = 0, {pi , pj } = 0, {qi , pj } = δij where {, } is the Poisson bracket:  X  ∂A ∂B ∂A ∂B − {A, B} = ∂qi ∂pi ∂pi ∂qi i The Hamiltonian of a Harmonic oscillator is given by H(x, p) = p2 /2m + 12 mω 2 x2 . With new coordinates p √ (θ, I), obtained by the canonical transformation x = 2I/mω cos(θ) and p = − 2Imω sin(θ), with inverse θ = arctan(−p/mωx) and I = p2 /2mω + 12 mωx2 it follows: H(θ, I) = ωI. The Hamiltonian of a charged particle with charge q in an external electromagnetic field is given by: H=

2 1  ~ + qV p~ − q A 2m

This Hamiltonian can be derived from the Hamiltonian of a free particle H = p2 /2m with the transformations ~ and H → H − qV . This is elegant from a relativistic point of view: this is equivalent to the p~ → p~ − q A transformation of the momentum 4-vector pα → pα − qAα . A gauge transformation on the potentials Aα corresponds with a canonical transformation, which make the Hamilton equations the equations of motion for the system.

1.7.3 Motion around an equilibrium, linearization For natural systems around equilibrium the following equations are valid:  2    ∂ V ∂V = 0 ; V (q) = V (0) + Vik qi qk with Vik = ∂qi 0 ∂qi ∂qk 0 With T = 12 (Mik q˙i q˙k ) one receives the set of equations M q¨ + V q = 0. If qi (t) = ai exp(iωt) is substituted, this set of equations has solutions if det(V − ω 2 M ) = 0. This leads to the eigenfrequencies of the problem: aT V ak . If the equilibrium is stable holds: ∀k that ωk2 > 0. The general solution is a superposition if ωk2 = Tk ak M ak eigenvibrations.

1.7.4 Phase space, Liouville’s equation In phase space holds: ∇=

X ∂ X ∂ , ∂qi i ∂pi i

!

 X  ∂ ∂H ∂ ∂H − so ∇ · ~v = ∂qi ∂pi ∂pi ∂qi i

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If the equation of continuity, ∂t % + ∇ · (%~v ) = 0 holds, this can be written as: {%, H} +

∂% =0 ∂t

For an arbitrary quantity A holds: ∂A dA = {A, H} + dt ∂t Liouville’s theorem can than be written as: d% = 0 ; or: dt

Z pdq = constant

1.7.5 Generating functions Starting with the coordinate transformation: 

Qi = Qi (qi , pi , t) Pi = Pi (qi , pi , t)

one can derive the following Hamilton equations with the new Hamiltonian K: ∂K dQi = ; dt ∂Pi

∂K dPi =− dt ∂Qi

Now, a distinction between 4 cases can be made: 1. If pi q˙i − H = Pi Qi − K(Pi , Qi , t) − pi =

dF1 (qi , Qi , t) , the coordinates follow from: dt

∂F1 ∂F1 dF1 ; Pi = ; K=H+ ∂qi ∂Qi dt

dF2 (qi , Pi , t) , the coordinates follow from: 2. If pi q˙i − H = −P˙ i Qi − K(Pi , Qi , t) + dt pi =

∂F2 ∂F2 ∂F2 ; Qi = ; K=H+ ∂qi ∂Pi ∂t

3. If −p˙ i qi − H = Pi Q˙ i − K(Pi , Qi , t) + qi = −

dF3 (pi , Qi , t) , the coordinates follow from: dt

∂F3 ∂F3 ∂F3 ; Pi = − ; K =H+ ∂pi ∂Qi ∂t

4. If −p˙ i qi − H = −Pi Qi − K(Pi , Qi , t) + qi = −

dF4 (pi , Pi , t) , the coordinates follow from: dt

∂F4 ∂F4 ∂F4 ; Qi = ; K=H+ ∂pi ∂pi ∂t

The functions F1 , F2 , F3 and F4 are called generating functions.

Chapter 2

Electricity & Magnetism 2.1 The Maxwell equations The classical electromagnetic field can be described by the Maxwell equations. Those can be written both as differential and integral equations: ZZ ~ = ρfree ~ · ~n )d2 A = Qfree,included ∇·D

(D ZZ ~ =0 ~ · ~n )d2 A = 0 ∇·B

(B I ~ ~ = − ∂B ~ · d~s = − dΦ ∇×E E dt ∂t I ~ dΨ ∂D ~ ~ ~ ∇ × H = Jfree + H · d~s = Ifree,included + dt ∂t ZZ ZZ ~ · ~n )d2 A. ~ · ~n )d2 A, Φ = (B For the fluxes holds: Ψ = (D ~ polarization P~ and electric field strength E ~ depend on each other according to: The electric displacement D, ~ + P~ = ε0 εr E, ~ P~ = ~ = ε0 E D

P

p0 /Vol, εr = 1 + χe , with χe = ~

np20 3ε0 kT

~ the magnetization M ~ and the magnetic flux density B ~ depend on each other The magnetic field strength H, according to: µ0 nm20 ~ M ~ = P m/Vol, ~ +M ~ ) = µ0 µr H, ~ = µ0 (H ~ µr = 1 + χm , with χm = B 3kT

2.2 Force and potential The force and the electric field between 2 point charges are given by: F~12 =

~ Q1 Q2 ~ = F ~er ; E 2 4πε0 εr r Q

The Lorentzforce is the force which is felt by a charged particle that moves through a magnetic field. The ~ ) = l(I~ × B ~ ). origin of this force is a relativistic transformation of the Coulomb force: F~L = Q(~v × B The magnetic field in point P which results from an electric current is given by the law of Biot-Savart, also known als the law of Laplace. In here, d~l k I~ and ~r points from d~l to P : ~P = dB

µ0 I ~ dl × ~er 4πr2

If the current is time-dependent one has to take retardation into account: the substitution I(t) → I(t − r/c) has to be applied. Z2 ~ · d~s and A ~ = 1B ~ × ~r. E 2

The potentials are given by: V12 = − 1

9

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Here, the freedom remains to apply a gauge transformation. The fields can be derived from the potentials as follows: ~ ~ = ∇×A ~ ~ = −∇V − ∂ A , B E ∂t ~ = ~v × E. ~ Further holds the relation: c2 B

2.3 Gauge transformations The potentials of the electromagnetic fields transform as follows when a gauge transformation is applied:  ~0 = A ~ − ∇f  A ∂f  V0 =V + ∂t ~ and B ~ do not change. This results in a canonical transformation of the Hamiltonian. Further, so the fields E the freedom remains to apply a limiting condition. Two common choices are: ~ and V : 2V = − ρ , ~ + 1 ∂V = 0. This separates the differential equations for A 1. Lorentz-gauge: ∇ · A 2 c ∂t ε0 ~ ~ = −µ0 J. 2A ~ = 0. If ρ = 0 and J~ = 0 holds V = 0 and follows A ~ from 2A ~ = 0. 2. Coulomb gauge: ∇ · A

2.4 Energy of the electromagnetic field The energy density of the electromagnetic field is:

Z Z dW = w = HdB + EdD dVol The energy density can be expressed in the potentials and currents as follows: Z Z ~ d3 x , wel = 1 ρV d3 x wmag = 12 J~ · A 2

2.5 Electromagnetic waves 2.5.1 Electromagnetic waves in vacuum The wave equation 2Ψ(~r, t) = −f (~r, t) has the general solution, with c = (ε0 µ0 )−1/2 : Z f (~r, t − |~r − ~r 0 |/c) 3 0 d r Ψ(~r, t) = 4π|~r − ~r 0 | ~ r , t) = J(~ ~ r ) exp(−iωt) and A(~ ~ r , t) = A(~ ~ r ) exp(−iωt) with: If this is written as: J(~ Z Z r − ~r 0 |) 3 0 1 r − ~r 0 |) 3 0 µ 0 exp(ik|~ 0 exp(ik|~ ~ ~ J(~r ) d ρ(~ r d ~r ~ r , V (~ r ) = ) A(~r ) = 4π |~r − ~r 0 | 4πε |~r − ~r 0 | A derivation via multipole expansion will show that for the radiated energy holds, if d, λ  r: Z 2 k2 dP 0 i~ k·~ r 3 0 = (~ r )e d r J ⊥ dΩ 32π 2 ε0 c The energy density of the electromagnetic wave of a vibrating dipole at a large distance is: p20 sin2 (θ)ω 4 ck 4 |~ p |2 , P = 2 2 4 32π ε0 r c 12πε0 ~ S ~=E ~ ×H ~ = cW~ev . The irradiance is the The radiated energy can be derived from the Poynting vector S: ~ |/c, ~ |it . The radiation pressure ps is given by ps = (1 + R)|S time-averaged of the Poynting vector: I = h|S where R is the coefficient of reflection. w = ε0 E 2 =

p20 sin2 (θ)ω 4 sin2 (kr − ωt) , 16π 2 ε0 r2 c4

hwit =

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11

2.5.2 Electromagnetic waves in matter The wave equations in matter, with cmat = (εµ)−1/2 the lightspeed in matter, are:     ∂2 µ ∂ ~ ∂2 µ ∂ ~ E =0, ∇2 − εµ 2 − B=0 ∇2 − εµ 2 − ∂t ρ ∂t ∂t ρ ∂t ~ = E exp(i(~k ·~r −ωt)) and B ~ = B exp(i(~k ·~r −ωt)) give, after substitution of monochromatic plane waves: E the dispersion relation: iµω k 2 = εµω 2 + ρ The first term arises from the displacement current, the second from the conductance current. If k is written in the form k := k 0 + ik 00 it follows that: v v s s u u q q u u 1 1 and k 00 = ω 12 εµt−1 + 1 + k 0 = ω 12 εµt1 + 1 + 2 (ρεω) (ρεω)2 ~ = E exp(−k 00~n ·~r ) exp(i(k 0~n ·~r − ωt)). If the material is a good conductor, This results in a damped wave: E r µω . the wave vanishes after approximately one wavelength, k = (1 + i) 2ρ

2.6 Multipoles ∞

Because

1X 1 = 0 |~r − ~r | r 0

 0 l r Q X kn Pl (cos θ) the potential can be written as: V = r 4πε n rn

For the lowest-order terms this results in: R • Monopole: l = 0, k0 = ρdV R • Dipole: l = 1, k1 = r cos(θ)ρdV P • Quadrupole: l = 2, k2 = 12 (3zi2 − ri2 ) i

~ ext , and 1. The electric dipole: dipole moment: p~ = Ql~e , where ~e goes from ⊕ to , and F~ = (~ p · ∇)E ~ out . W = −~ p·E   Q 3~ p · ~r ~ out ~ − p~ . The torque is: ~τ = ~p × E Electric field: E ≈ 4πεr3 r2 √ ~ out 2. The magnetic dipole: dipole moment: if r  A: ~µ = I~ × (A~e⊥ ), F~ = (~µ · ∇)B 2 mv⊥ ~ out , W = −~ µ×B |µ| = 2B   −µ 3µ · ~r ~ ~ out Magnetic field: B = −µ ~ . The moment is: ~τ = ~µ × B 4πr3 r2

2.7 Electric currents The continuity equation for charge is:

∂ρ + ∇ · J~ = 0. The electric current is given by: ∂t ZZ dQ = (J~ · ~n )d2 A I= dt

~ For most conductors holds: J~ = E/ρ, where ρ is the resistivity.

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dΦ . If the current If the flux enclosed by a conductor changes this results in an induced voltage Vind = −N dt flowing through a conductor changes, this results in a self-inductance which opposes the original change: dI Vselfind = −L . If a conductor encloses a flux Φ holds: Φ = LI. dt µN I where l is the length, R the radius The magnetic induction within a coil is approximated by: B = √ 2 l + 4R2 and N the number of coils. The energy contained within a coil is given by W = 12 LI 2 and L = µN 2 A/l. The capacity is defined by: C = Q/V . For a capacitor holds: C = ε0 εr A/d where d is the distance between the plates and A the surface of one plate. The electric field strength between the plates is E = σ/ε0 = Q/ε0 A where σ is the surface charge. The accumulated energy is given by W = 12 CV 2 . The current through a dV . capacity is given by I = −C dt For most PTC resistors holds approximately: R = R0 (1 + αT ), where R0 = ρl/A. For a NTC holds: R(T ) = C exp(−B/T ) where B and C depend only on the material. If a current flows through two different, connecting conductors x and y, the contact area will heat up or cool down, depending on the direction of the current: the Peltier effect. The generated or removed heat is given by: W = Πxy It. This effect can be amplified with semiconductors. The thermic voltage between 2 metals is given by: V = γ(T − T0 ). For a Cu-Konstantane connection holds: γ ≈ 0.2 − 0.7 mV/K. P In an electrical net with only In = 0, P currents, Kirchhoff’s equations apply: for a knot holds: P stationary along a closed path holds: Vn = In Rn = 0.

2.8 Depolarizing field If a dielectric material is placed in an electric or magnetic field, the field strength within and outside the material will change because the material will be polarized or magnetized. If the medium has an ellipsoidal ~ 0 then the depolarizing is field ~ 0 or B shape and one of the principal axes is parallel with the external field E homogeneous. ~ ~ mat − E ~0 = − N P ~ dep = E E ε0 ~ ~ ~ ~ Hdep = Hmat − H0 = −N M N is a constant depending only on the shape of the object placed in the field, with 0 ≤ N ≤ 1. For a few limiting cases of an ellipsoid holds: a thin plane: N = 1, a long, thin bar: N = 0, a sphere: N = 13 .

2.9 Mixtures of materials The average electric displacement in a material which is inhomogenious on a mesoscopic scale is given by: −1  φ2 (1 − x) where x = ε1 /ε2 . For a sphere holds: Φ = hDi = hεEi = ε∗ hEi where ε∗ = ε1 1 − Φ(ε∗ /ε2 ) 1 2 3 + 3 x. Further holds: !−1 X X φi ≤ ε∗ ≤ φi εi εi i i

Chapter 3

Relativity 3.1 Special relativity 3.1.1 The Lorentz transformation The Lorentz transformation (~x 0 , t0 ) = (~x 0 (~x, t), t0 (~x, t)) leaves the wave equation invariant if c is invariant: ∂2 ∂2 1 ∂2 ∂2 ∂2 ∂2 1 ∂2 ∂2 + + − = + + − ∂x2 ∂y 2 ∂z 2 c2 ∂t2 ∂x02 ∂y 02 ∂z 02 c2 ∂t02 This transformation can also be found when ds2 = ds02 is demanded. The general form of the Lorentz transformation is given by:   (γ − 1)(~x · ~v )~v ~x · ~v 0 0 − γ~v t , t = γ t − 2 ~x = ~x + |v|2 c where

1 γ=r 2 1 − v2 c

The velocity difference ~v 0 between two observers transforms according to:   −1   ~v1 · ~v2 ~v1 · ~v2 ~v2 + (γ − 1) 2 ~v1 − γ~v1 ~v = γ 1 − c2 v1 0

If the velocity is parallel to the x-axis, this becomes y 0 = y, z 0 = z and: x0 = γ(x − vt) , x = γ(x0 + vt0 )    xv  x0 v v2 − v1 0 0 t =γ t− 2 , t=γ t + 2 , v0 = v1 v2 c c 1− 2 c If ~v = v~ex holds: p0x

  βW , W 0 = γ(W − vpx ) = γ px − c

With β = v/c the electric field of a moving charge is given by: ~ = E

(1 − β 2 )~er Q 4πε0 r2 (1 − β 2 sin2 (θ))3/2

The electromagnetic field transforms according to: ~0

~0

~ + ~v × B ~) , B =γ E = γ(E

~ ~ − ~v × E B 2 c

!

Length, mass and time transform according to: ∆tr = γ∆t0 , mr = γm0 , lr = l0 /γ, with 0 the quantities in a co-moving reference frame and r the quantities in a frame moving with velocity v w.r.t. it. The proper time τ is defined as: dτ 2 = ds2 /c2 , so ∆τ = ∆t/γ. For energy and momentum holds: W = mr c2 = γW0 , 13

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W 2 = m20 c4 + p2 c2 . p = mr v = γm0 v = W v/c2 , and pc = W β where β = v/c. The force is defined by F~ = d~ p/dt. 4-vectors have the property that their modulus is independent of the observer: their components can change after a coordinate transformation but not their modulus. The difference of two 4-vectors transforms also as dxα α . The relation with the “common” velocity a 4-vector. The 4-vector for the velocity is given by U = dτ i i α i u := dx /dt is: U = (γu , icγ). For particles with nonzero restmass holds: U α Uα = −c2 , for particles with zero restmass (so with v = c) holds: U α Uα = 0. The 4-vector for energy and momentum is given by: pα = m0 U α = (γpi , iW/c). So: pα pα = −m20 c2 = p2 − W 2 /c2 .

3.1.2 Red and blue shift There are three causes of red and blue shifts:

  v cos(ϕ) f0 =γ 1− . f c This can give both red- and blueshift, also ⊥ to the direction of motion.

1. Motion: with ~ev · ~er = cos(ϕ) follows:

2. Gravitational redshift:

κM ∆f = 2. f rc

3. Redshift because the universe expands, resulting in e.g. the cosmic background radiation: R0 λ0 = . λ1 R1

3.1.3 The stress-energy tensor and the field tensor The stress-energy tensor is given by: Tµν = (%c2 + p)uµ uν + pgµν +


1 Fµα Fνα + 14 gµν F αβ Fαβ 2 c

The conservation laws can than be written as: ∇ν T µν = 0. The electromagnetic field tensor is given by: Fαβ =

∂Aβ ∂Aα − α ∂x ∂xβ

~ iV /c) and Jµ := (J, ~ icρ). The Maxwell equations can than be written as: with Aµ := (A, ∂ν F µν = µ0 J µ , ∂λ Fµν + ∂µ Fνλ + ∂ν Fλµ = 0 The equations of motion for a charged particle in an EM field become with the field tensor: dpα = qFαβ uβ dτ

3.2 General relativity 3.2.1 Riemannian geometry, the Einstein tensor The basic principles of general relativity are: 1. The geodesic postulate: free falling particles move along geodesics of space-time with the proper time τ or arc length s as parameter. For particles with Rzero rest mass (photons), the use of a free parameter is required because for them holds ds = 0. From δ ds = 0 the equations of motion can be derived: β γ d2 xα α dx dx =0 + Γ βγ ds2 ds ds

Chapter 3: Relativity

15

2. The principle of equivalence: inertial mass ≡ gravitational mass ⇒ gravitation is equivalent with a curved space-time were particles move along geodesics. 3. By a proper choice of the coordinate system it is possible to make the metric locally flat in each point xi : gαβ (xi ) = ηαβ :=diag(−1, 1, 1, 1). µ T ν := ∇α ∇β T µ − ∇β ∇α T µ , where the covariant derivative is given The Riemann tensor is defined as: Rναβ by ∇j ai = ∂j ai + Γijk ak and ∇j ai = ∂j ai − Γkij ak . Here,   ∂gj k g il ∂glj ∂glk ∂ 2 x¯l ∂xi i i + − = , Γjk = , for Euclidean spaces this reduces to: Γ jk 2 ∂xk ∂xj ∂xl ∂xj ∂xk ∂ x ¯l µ σ Tνσ + Rναβ Tσµ , ∇k aij = are the Christoffel symbols. For a second-order tensor holds: [∇α , ∇β ]Tνµ = Rσαβ j il i l i i l l l ij ij i lj ∂k aj − Γkj al + Γkl aj , ∇k aij = ∂k aij − Γki alj − Γkj ajl and ∇k a = ∂k a + Γkl a + Γkl a . The following α α α σ α σ = ∂µ Γα holds: Rβµν βν − ∂ν Γβµ + Γσµ Γβν − Γσν Γβµ . µ , which is symmetric: Rαβ = Rβα . The Ricci tensor is a contraction of the Riemann tensor: Rαβ := Rαµβ The Bianchi identities are: ∇λ Rαβµν + ∇ν Rαβλµ + ∇µ Rαβνλ = 0. α is the Ricci scalar, for which The Einstein tensor is given by: Gαβ := Rαβ − 12 g αβ R, where R := Rα p R 2 holds: ∇β Gαβ = 0. With the variational principle δ (L(gµν ) − Rc /16πκ) |g|d4 x = 0 for variations gµν → gµν + δgµν the Einstein field equations can be derived:

Gαβ =

8πκ Tαβ c2

, which can also be written as Rαβ =

8πκ (Tαβ − 12 gαβ Tµµ ) c2

For empty space this is equivalent to Rαβ = 0. The equation Rαβµν = 0 has as only solution a flat space. The Einstein equations are 10 independent equations, which are of second order in gµν . From this, the Laplace equation from Newtonian gravitation can be derived by stating: gµν = ηµν + hµν , where |h|  1. In the stationary case, this results in ∇2 h00 = 8πκ%/c2 . 8πκ Tαβ c2 where Λ is the cosmological constant. This constant plays a role in inflatory models of the universe.

The most general form of the field equations is: Rαβ − 12 gαβ R + Λgαβ =

3.2.2 The line element The metric tensor in an Euclidean space is given by: gij =

X ∂x ¯k ∂ x ¯k . i ∂x ∂xj k

In general holds: ds = gµν dx dx . In special relativity this becomes ds2 = −c2 dt2 + dx2 + dy 2 + dz 2 . This metric, ηµν :=diag(−1, 1, 1, 1), is called the Minkowski metric. 2

µ

ν

The external Schwarzschild metric applies in vacuum outside a spherical mass distribution, and is given by:    −1 2m 2 2 2m 2 dr2 + r2 dΩ2 c dt + 1 − ds = −1 + r r Here, m := M κ/c2 is the geometrical mass of an object with mass M , and dΩ2 = dθ2 + sin2 θdϕ2 . This metric is singular for r = 2m = 2κM/c2 . If an object is smaller than its event horizon 2m, that implies that its escape velocity is > c, it is called a black hole. The Newtonian limit of this metric is given by: ds2 = −(1 + 2V )c2 dt2 + (1 − 2V )(dx2 + dy 2 + dz 2 ) where V = −κM/r is the Newtonian gravitation potential. In general relativity, the components of gµν are associated with the potentials and the derivatives of gµν with the field strength. The Kruskal-Szekeres coordinates are used to solve certain problems with the Schwarzschild metric near r = 2m. They are defined by:

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• r > 2m:

   u         v

• r < 2m:

   u         v

r

 r  r − 1 exp cosh 2m 4m



r

 r  r − 1 exp sinh 2m 4m



 r  r exp sinh 1− 2m 4m



=

= r =

=

t 4m

t 4m t 4m

 



r    r  t r exp cosh 1− 2m 4m 4m

• r = 2m: here, the Kruskal coordinates are singular, which is necessary to eliminate the coordinate singularity there. The line element in these coordinates is given by: ds2 = −

32m3 −r/2m 2 e (dv − du2 ) + r2 dΩ2 r

The line r = 2m corresponds to u = v = 0, the limit x0 → ∞ with u = v and x0 → −∞ with u = −v. The Kruskal coordinates are only singular on the hyperbole v 2 − u2 = 1, this corresponds with r = 0. On the line dv = ±du holds dθ = dϕ = ds = 0. For the metric outside a rotating, charged spherical mass the Newman metric applies:     r2 + a2 cos2 θ 2mr − e2 2 2 2 1− 2 c dt − dr2 − (r2 + a2 cos2 θ)dθ2 − ds = r + a2 cos2 θ r2 − 2mr + a2 − e2     2a(2mr − e2 ) (2mr − e2 )a2 sin2 θ 2 2 2 2 sin θdϕ + sin2 θ(dϕ)(cdt) r +a + r2 + a2 cos2 θ r2 + a2 cos2 θ where m = κM/c2 , a = L/M c and e = κQ/ε0 c2 . √ A rotating charged black hole has an event horizon with RS = m + m2 − a2 − e2 . Near rotating black holes frame dragging occurs because gtϕ 6= 0. For the Kerr metric (e = 0, a 6= 0) then √ follows that within the surface RE = m + m2 − a2 cos2 θ (de ergosphere) no particle can be at rest.

3.2.3 Planetary orbits and the perihelion shift

R ToR find a planetary orbit, the variational problem δ ds = 0 has to be solved. This is equivalent to the problem R δ ds2 = δ gij dxi dxj = 0. Substituting the external Schwarzschild metric yields for a planetary orbit:   m du  du d2 u 3mu + + u = dϕ dϕ2 dϕ h2 where u := 1/r and h = r2 ϕ˙ =constant. The term 3mu is not present  in the classical solution. This term can h2 κM 1+ 2 . in the classical case also be found from a potential V (r) = − r r The orbital equation gives r =constant as solution, or can, after dividing by du/dϕ, be solved with perturbation theory. In zeroth order, this results in an elliptical orbit: u0 (ϕ) = A + B cos(ϕ) with A = m/h2 and B an arbitrary constant. In first order, this becomes:   B2 B2 − cos(2ϕ) u1 (ϕ) = A + B cos(ϕ − εϕ) + ε A + 2A 6A where ε = 3m2 /h2 is small. The perihelion of a planet is the point for which r is minimal, or u maximal. This is the case if cos(ϕ − εϕ) = 0 ⇒ ϕ ≈ 2πn(1 + ε). For the perihelion shift then follows: ∆ϕ = 2πε = 6πm2 /h2 per orbit.

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17

3.2.4 The trajectory of a photon For the trajectory of a photon (and for each particle with zero restmass) holds ds2 = 0. Substituting the external Schwarzschild metric results in the following orbital equation:   du d2 u + u − 3mu = 0 dϕ dϕ2

3.2.5 Gravitational waves Starting with the approximation gµν = ηµν + hµν for weak gravitational fields and the definition h0µν = 0 0 ν hµν − 12 ηµν hα α it follows that 2hµν = 0 if the gauge condition ∂hµν /∂x = 0 is satisfied. From this, it follows that the loss of energy of a mechanical system, if the occurring velocities are  c and for wavelengths  the size of the system, is given by:  2 G X d3 Qij dE =− 5 dt 5c i,j dt3 with Qij =

R

%(xi xj − 13 δij r2 )d3 x the mass quadrupole moment.

3.2.6 Cosmology If for the universe as a whole is assumed: 1. There exists a global time coordinate which acts as x0 of a Gaussian coordinate system, 2. The 3-dimensional spaces are isotrope for a certain value of x0 , 3. Each point is equivalent to each other point for a fixed x0 . then the Robertson-Walker metric can be derived for the line element: ds2 = −c2 dt2 +

R2 (t) 2 2   2 2 (dr + r dΩ ) kr r02 1 − 2 4r0

For the scalefactor R(t) the following equations can be derived: ¨ R˙ 2 + kc2 R˙ 2 + kc2 8πκp 8πκ% Λ 2R + + = − + Λ and = 2 2 2 R R c R 3 3 where p is the pressure and % the density of the universe. If Λ = 0 can be derived for the deceleration parameter q: ¨ 4πκ% RR = q=− 2 ˙ 3H 2 R ˙ where H = R/R is Hubble’s constant. This is a measure of the velocity with which galaxies far away are moving away from each other, and has the value ≈ (75 ± 25) km·s−1 ·Mpc−1 . This gives 3 possible conditions for the universe (here, W is the total amount of energy in the universe): 1. Parabolical universe: k = 0, W = 0, q = 12 . The expansion velocity of the universe → 0 if t → ∞. The hereto related critical density is %c = 3H 2 /8πκ. 2. Hyperbolical universe: k = −1, W < 0, q < positive forever.

1 2.

The expansion velocity of the universe remains

3. Elliptical universe: k = 1, W > 0, q > 12 . The expansion velocity of the universe becomes negative after some time: the universe starts collapsing.

Chapter 4

Oscillations 4.1 Harmonic oscillations ˆ i(ωt±ϕ) ≡ Ψ ˆ cos(ωt ± ϕ), The general form of a harmonic oscillation is: Ψ(t) = Ψe ˆ is the amplitude. A superposition of several harmonic oscillations with the same frequency results in where Ψ another harmonic oscillation: X ˆ i cos(αi ± ωt) = Φ ˆ cos(β ± ωt) Ψ i

with:

P

ˆ i sin(αi ) Ψ

i

ˆ2 = and Φ tan(β) = P ˆ i cos(αi ) Ψ i

For harmonic oscillations holds:

Z x(t)dt =

X

ˆ2 + 2 Ψ i

i

XX j>i

ˆ iΨ ˆ j cos(αi − αj ) Ψ

i

dn x(t) x(t) and = (iω)n x(t). iω dtn

4.2 Mechanic oscillations For a construction with a spring with constant C parallel to a damping k which is connected to a mass M , to which a periodic force F (t) = Fˆ cos(ωt) is applied holds the equation of motion m¨ x = F (t) − k x˙ − Cx. With complex amplitudes, this becomes −mω 2 x = F − Cx − ikωx. With ω02 = C/m follows: x=

F F , and for the velocity holds: x˙ = √ m(ω02 − ω 2 ) + ikω i Cmδ + k

ω0 ω − . The quantity Z = F/x˙ is called the impedance of the system. The quality of the system ω0 √ω Cm . is given by Q = k The frequency √ with minimal |Z| is called velocity resonance frequency. This is equal to ω0 . In the resonance curve |Z|/ √ Cm is plotted against ω/ω0 . The width of this curve is characterized by the points where |Z(ω)| = |Z(ω0 )| 2. In these points holds: R = X and δ = ±Q−1 , and the width is 2∆ωB = ω0 /Q. where δ =

The stiffness of an oscillating system is given by F/x.qThe amplitude resonance frequency ωA is the frequency where iωZ is minimal. This is the case for ωA = ω0

1 − 12 Q2 .

The dampingrfrequency ωD is a measure for the time in which an oscillating system comes to rest. It is given 1 . A weak damped oscillation (k 2 < 4mC) dies out after TD = 2π/ωD . For a critical by ωD = ω0 1 − 4Q2 damped oscillation (k 2 = 4mC) holds ωD = 0. A strong damped oscillation (k 2 > 4mC) drops like (if k 2  4mC) x(t) ≈ x0 exp(−t/τ ).

4.3 Electric oscillations The impedance is given by: Z = R + iX. The phase angle is ϕ := arctan(X/R). The impedance of a resistor is R, of a capacitor 1/iωC and of a self inductor iωL. The quality of a coil is Q = ωL/R. The total impedance in case several elements are positioned is given by: 18

Chapter 4: Oscillations

19

1. Series connection: V = IZ, Ztot =

X

Zi , Ltot =

i

X

Li ,

i

X 1 1 Z0 , Z = R(1 + iQδ) = , Q= Ctot C R i i

2. parallel connection: V = IZ, X 1 X 1 X 1 R R 1 = , = , Ctot = Ci , Q = , Z= Ztot Zi Ltot Li Z0 1 + iQδ i i i r Here, Z0 =

1 L . and ω0 = √ C LC

The power given by a source is given by P (t) = V (t) · I(t), so hP it = Vˆeff Iˆeff cos(∆φ) = 12 Vˆ Iˆ cos(φv − φi ) = 12 Iˆ2 Re(Z) = 12 Vˆ 2 Re(1/Z), where cos(∆φ) is the work factor.

4.4 Waves in long conductors r These cables are in use for signal transfer, e.g. coax cable. For them holds: Z0 = r dx dx . The transmission velocity is given by v = dL dC

dL dx . dx dC

4.5 Coupled conductors and transformers For two coils enclosing each others flux holds: if Φ12 is the part of the flux originating from I2 through coil 2 which is enclosed by coil 1, than holds Φ12 = M12 I2 , Φ21 = M21 I1 . For the coefficients of mutual induction Mij holds: p N 1 Φ1 N 2 Φ2 = ∼ N1 N2 M12 = M21 := M = k L1 L2 = I2 I1 where 0 ≤ k ≤ 1 is the coupling factor. For a transformer is k ≈ 1. At full load holds: r I2 iωM N1 L1 V1 = =− ≈− =− V2 I1 iωL2 + Rload L2 N2

4.6 Pendulums The oscillation time T = 1/f , and for different types of pendulums is given by: p • Oscillating spring: T = 2π m/C if the spring force is given by F = C · ∆l. p • Physical pendulum: T = 2π I/τ with τ the moment of force and I the moment of inertia. • Torsion pendulum: T = 2π

p I/κ with κ =

• Mathematical pendulum: T = 2π lum.

2lm the constant of torsion and I the moment of inertia. πr4 ∆ϕ

p l/g with g the acceleration of gravity and l the length of the pendu-

Chapter 5

Waves 5.1 The wave equation The general form of the wave equation is: 2u = 0, or: ∇2 u −

1 ∂2u ∂2u ∂2u ∂2u 1 ∂2u = + + − =0 v 2 ∂t2 ∂x2 ∂y 2 ∂z 2 v 2 ∂t2

where u is the disturbance and v the propagation velocity. In general holds: v = f λ. By definition holds: kλ = 2π and ω = 2πf . In principle, there are two types of waves: 1. Longitudinal waves: for these holds ~k k ~v k ~u. 2. Transversal waves: for these holds ~k k ~v ⊥ ~u. The phase velocity is given by vph = ω/k. The group velocity is given by:   dω dvph k dn = vph + k = vph 1 − vg = dk dk n dk where n is the refractive index of the medium. If vph does not depend on ω holds: vph = vg . In a dispersive medium it is possible that vg > vph or vg < vph , and vg · vf = c2 . If one wants to transfer information with a wave, e.g. by modulation of an EM wave, the information travels with the velocity at with a change in the electromagnetic field propagates. This velocity is often almost equal to the group velocity. For some media, the propagation velocity follows from: p • Pressure waves in a liquid or gas: v = κ/%, where κ is the modulus of compression. p p • For pressure waves in a gas also holds: v = γp/% = γRT /M. p • Pressure waves in a thin solid bar with diameter << λ: v = E/% p • waves in a string: v = Fspan l/m s    2πh gλ 2πγ + tanh • Surface waves on a liquid: v = 2π %λ λ √ where h is the depth of the liquid and γ the surface tension. If h  λ holds: v ≈ gh.

5.2 Solutions of the wave equation 5.2.1 Plane waves In n dimensions a harmonic plane wave is defined by: ˆ cos(ωt) u(~x, t) = 2n u

n X i=1

20

sin(ki xi )

Chapter 5: Waves

21

The equation for a harmonic traveling plane wave is: u(~x, t) = u ˆ cos(~k · ~x ± ωt + ϕ) If waves reflect at the end of a spring this will result in a change in phase. A fixed end gives a phase change of π/2 to the reflected wave, with boundary condition u(l) = 0. A lose end gives no change in the phase of the reflected wave, with boundary condition (∂u/∂x)l = 0. If an observer is moving w.r.t. the wave with a velocity vobs , he will observe a change in frequency: the vf − vobs f = . Doppler effect. This is given by: f0 vf

5.2.2 Spherical waves When the situation is spherical symmetric, the homogeneous wave equation is given by: 1 ∂ 2 (ru) ∂ 2 (ru) − =0 v 2 ∂t2 ∂r2 with general solution: u(r, t) = C1

f (r − vt) g(r + vt) + C2 r r

5.2.3 Cylindrical waves When the situation has a cylindrical symmetry, the homogeneous wave equation becomes:   1 ∂2u 1 ∂ ∂u − r =0 v 2 ∂t2 r ∂r ∂r This is a Bessel equation, with solutions which can be written as Hankel functions. For sufficient large values of r these are approximated by: u ˆ u(r, t) = √ cos(k(r ± vt)) r

5.2.4 The general solution in one dimension Starting point is the equation:

 N  X ∂m ∂ 2 u(x, t) = bm m u(x, t) ∂t2 ∂x m=0

where bm ∈ IR. Substituting u(x, t) = Aei(kx−ωt) gives two solutions ωj = ωj (k) as dispersion relations. The general solution is given by: Z∞   a(k)ei(kx−ω1 (k)t) + b(k)ei(kx−ω2 (k)t) dk u(x, t) = −∞

Because in general the frequencies ωj are non-linear in k there is dispersion and the solution cannot be written any more as a sum of functions depending only on x ± vt: the wave front transforms.

5.3 The stationary phase method Usually the Fourier integrals of the previous section cannot be calculated exactly. If ωj (k) ∈ IR the stationary phase method can be applied. Assuming that a(k) is only a slowly varying function of k, one can state that the parts of the k-axis where the phase of kx − ω(k)t changes rapidly will give no net contribution to the integral because the exponent oscillates rapidly there. The only areas contributing significantly to the integral are areas d (kx − ω(k)t) = 0. Now the following approximation is possible: with a stationary phase, determined by dk v Z∞ N u X   u 2π a(k)ei(kx−ω(k)t) dk ≈ t d2 ω(k ) exp −i 41 π + i(ki x − ω(ki )t) −∞

i=1

dki2

i

Physics Formulary by ir. J.C.A. Wevers

22

5.4 Green functions for the initial-value problem This method is preferable if the solutions deviate much from the stationary solutions, like point-like excitations. Starting with the wave equation in one dimension, with ∇2 = ∂ 2 /∂x2 holds: if Q(x, x0 , t) is the solution with ∂Q(x, x0 , 0) = 0, and P (x, x0 , t) the solution with initial values initial values Q(x, x0 , 0) = δ(x − x0 ) and ∂t ∂P (x, x0 , 0) = δ(x − x0 ), then the solution of the wave equation with arbitrary initial P (x, x0 , 0) = 0 and ∂t ∂u(x, 0) is given by: conditions f (x) = u(x, 0) and g(x) = ∂t Z∞

0

0

0

Z∞

f (x )Q(x, x , t)dx +

u(x, t) = −∞

g(x0 )P (x, x0 , t)dx0

−∞

P and Q are called the propagators. They are defined by: Q(x, x0 , t) = 0

P (x, x , t) = Further holds the relation: Q(x, x0 , t) =

1 2 [δ(x

( 1 2v 0

− x0 − vt) + δ(x − x0 + vt)] if |x − x0 | < vt if |x − x0 | > vt

∂P (x, x0 , t) ∂t

5.5 Waveguides and resonating cavities The boundary conditions for a perfect conductor can be derived from the Maxwell equations. If ~n is a unit ~ is a surface current density, than holds: vector ⊥ the surface, pointed from 1 to 2, and K ~ 1) = σ ~2 −D ~n · (D ~ ~ ~n · (B2 − B1 ) = 0

~2 − E ~ 1) = 0 ~n × (E ~ ~ 1) = K ~ ~n × (H2 − H

~ x, t) = ~ x, t) = E(x, ~ y)ei(kz−ωt) and B(~ In a waveguide holds because of the cylindrical symmetry: E(~ i(kz−ωt) ~ B(x, y)e . From this one can now deduce that, if Bz and Ez are not ≡ 0:     ∂Ez ∂Ez i i ∂Bz ∂Bz − εµω B + εµω = k k Bx = y εµω 2 − k 2  ∂x ∂y  εµω 2 − k 2  ∂y ∂x  ∂Bz ∂Bz i i ∂Ez ∂Ez + εµω − εµω Ey = k k Ex = εµω 2 − k 2 ∂x ∂y εµω 2 − k 2 ∂y ∂x Now one can distinguish between three cases: 1. Bz ≡ 0: the Transversal Magnetic modes (TM). Boundary condition: Ez |surf = 0. ∂Bz = 0. 2. Ez ≡ 0: the Transversal Electric modes (TE). Boundary condition: ∂n surf For the TE and TM modes this gives an eigenvalue problem for Ez resp. Bz with boundary conditions:   2 ∂ ∂2 + 2 ψ = −γ 2 ψ with eigenvalues γ 2 := εµω 2 − k 2 ∂x2 ∂y p This gives a discrete solution ψ` with eigenvalue γ`2 : k = εµω 2 − γ`2 . For ω < ω` , k is imaginary and the wave is damped. Therefore, ω` is called the cut-off frequency. In rectangular conductors the following expression can be found for the cut-off frequency for modes TEm,n of TMm,n : 2 λ` = p (m/a)2 + (n/b)2

Chapter 5: Waves

23

3. Ez and Bz are zero everywhere: the Transversal electromagnetic mode (TEM). Than holds: k = √ ±ω εµ and vf = vg , just as if here were no waveguide. Further k ∈ IR, so there exists no cut-off frequency. In a rectangular, 3 dimensional resonating cavity with edges a, b and c the possible wave numbers are given n1 π n2 π n3 π , ky = , kz = This results in the possible frequencies f = vk/2π in the cavity: by: kx = a b c r n2y n2z v n2x + + f= 2 a2 b2 c2 For a cubic cavity, with a = b = c, the possible number of oscillating modes NL for longitudinal waves is given by: 4πa3 f 3 NL = 3v 3 Because transversal waves have two possible polarizations holds for them: NT = 2NL .

5.6 Non-linear wave equations The Van der Pol equation is given by: dx d2 x + ω02 x = 0 − εω0 (1 − βx2 ) dt2 dt βx2 can be ignored for very small values of the amplitude. Substitution of x ∼ eiωt gives: ω = 12 ω0 (iε ± q 2 1 − 12 ε2 ). The lowest-order instabilities grow as 12 εω0 . While x is growing, the 2nd term becomes larger and diminishes the growth. Oscillations on a time scale ∼ ω0−1 can exist. If x is expanded as x = x(0) + εx(1) + ε2 x(2) + · · · and this is substituted one obtains, besides periodic, secular terms ∼ εt. If it is assumed that there exist timescales τn , 0 ≤ τ ≤ N with ∂τn /∂t = εn and if the secular terms are put 0 one obtains: (   )  2 2 dx d 1 dx 2 1 2 2 + 2 ω0 x = εω0 (1 − βx ) dt 2 dt dt This is an energy equation. Energy is conserved if the left-hand side is 0. If x2 > 1/β, the right-hand side changes sign and an increase in energy changes into a decrease of energy. This mechanism limits the growth of oscillations. The Korteweg-De Vries equation is given by: ∂u ∂3u ∂u ∂u + − au + b2 3 = 0 ∂t ∂x | {z∂x} ∂x } | {z non−lin

dispersive

This equation is for example a model for ion-acoustic waves in a plasma. For this equation, soliton solutions of the following form exist: −d u(x − ct) = cosh2 (e(x − ct)) with c = 1 + 13 ad and e2 = ad/(12b2 ).

Chapter 6

Optics 6.1 The bending of light For the refraction at a surface holds: ni sin(θi ) = nt sin(θt ) where n is the refractive index of the material. Snell’s law is: λ1 v1 n2 = = n1 λ2 v2 If ∆n ≤ 1, the change in phase of the light is ∆ϕ = 0, if ∆n > 1 holds: ∆ϕ = π. The refraction of light in a material is caused by scattering from atoms. This is described by: n2 = 1 +

ne e 2 X fj 2 − ω 2 − iδω ε0 m j ω0,j

where ne is the electron density and fj the oscillator strength, for which holds:

P

fj = 1. From this follows

j

that vg = c/(1 + (ne e2 /2ε0 mω 2 )). From this the equation of Cauchy can be derived: n = a0 + a1 /λ2 . More n X ak . general, it is possible to expand n as: n = λ2k k=0

For an electromagnetic wave in general holds: n =

√ εr µr .

The path, followed by a light ray in material can be found from Fermat’s principle: Z2

Z2 dt = δ

δ 1

n(s) ds = 0 ⇒ δ c

1

Z2 n(s)ds = 0 1

6.2 Paraxial geometrical optics 6.2.1 Lenses The Gaussian lens formula can be deduced from Fermat’s principle with the approximations cos ϕ = 1 and sin ϕ = ϕ. For the refraction at a spherical surface with radius R holds: n2 n1 − n2 n1 − = v b R where |v| is the distance of the object and |b| the distance of the image. Applying this twice results in: 1 = (nl − 1) f



1 1 − R2 R1



where nl is the refractive index of the lens, f is the focal length and R1 and R2 are the curvature radii of both surfaces. For a double concave lens holds R1 < 0, R2 > 0, for a double convex lens holds R1 > 0 and R2 < 0. Further holds: 1 1 1 = − f v b 24

Chapter 6: Optics

25

D := 1/f is called the dioptric power of a lens. For a lens with thickness d and diameter D holds to a good approximation: 1/f = 8(n − 1)d/D2 . For two lenses placed on a line with distance d holds: 1 1 d 1 = + − f f1 f2 f1 f2 In these equations the following signs are being used for refraction at a spherical surface, as is seen by an incoming light ray: Quantity R f v b

+ Concave surface Converging lens Real object Virtual image

− Convex surface Diverging lens Virtual object Real image

6.2.2 Mirrors For images of mirrors holds: 1 1 2 h2 1 = + = + f v b R 2



1 1 − R v

2

where h is the perpendicular distance from the point the light ray hits the mirror to the optical axis. Spherical aberration can be reduced by not using spherical mirrors. A parabolical mirror has no spherical aberration for light rays parallel with the optical axis and is therefore often used for telescopes. The used signs are: Quantity R f v b

+ Concave mirror Concave mirror Real object Real image

− Convex mirror Convex mirror Virtual object Virtual image

6.2.3 Principal planes The nodal points N of a lens are defined by the figure on the right. If the lens is surrounded by the same medium on both sides, the nodal points are the same as the principal points H. The plane ⊥ the optical axis through the principal points is called the principal plane. If the lens is described by a matrix mij than for the distances h1 and h2 to the boundary of the lens holds: h1 = n

N1 r r r O N2

m11 − 1 m22 − 1 , h2 = n m12 m12

6.2.4 Magnification The linear magnification is defined by: N = −

b v

The angular magnification is defined by: Nα = −

αsyst αnone

where αsys is the size of the retinal image with the optical system and αnone the size of the retinal image without the system. Further holds: N · Nα = 1. For a telescope holds: N = fobjective /focular. The f-number is defined by f /Dobjective.

Physics Formulary by ir. J.C.A. Wevers

26

6.3 Matrix methods A light ray can be described by a vector (nα, y) with α the angle with the optical axis and y the distance to the optical axis. The change of a light ray interacting with an optical system can be obtained using a matrix multiplication:     n1 α1 n2 α2 =M y2 y1 where Tr(M ) = 1. M is a product of elementary matrices. These are:   1 0 1. Transfer along length l: MR = l/n 1   1 −D 2. Refraction at a surface with dioptric power D: MT = 0 1

6.4 Aberrations Lenses usually do not give a perfect image. Some causes are: 1. Chromatic aberration is caused by the fact that n = n(λ). This can be partially corrected with a lens which is composed of more lenses with different functions ni (λ). Using N lenses makes it possible to obtain the same f for N wavelengths. 2. Spherical aberration is caused by second-order effects which are usually ignored; a spherical surface does not make a perfect lens. Incomming rays far from the optical axis will more bent. 3. Coma is caused by the fact that the principal planes of a lens are only flat near the principal axis. Further away of the optical axis they are curved. This curvature can be both positive or negative. 4. Astigmatism: from each point of an object not on the optical axis the image is an ellipse because the thickness of the lens is not the same everywhere. 5. Field curvature can be corrected by the human eye. 6. Distorsion gives abberations near the edges of the image. This can be corrected with a combination of positive and negative lenses.

6.5 Reflection and transmission If an electromagnetic wave hits a transparent medium part of the wave will reflect at the same angle as the incident angle, and a part will be refracted at an angle according to Snell’s law. It makes a difference whether ~ field of the wave is ⊥ or k w.r.t. the surface. When the coefficients of reflection r and transmission t are the E defined as:         E0r E0r E0t E0t , r⊥ ≡ , tk ≡ , t⊥ ≡ rk ≡ E0i k E0i ⊥ E0i k E0i ⊥ where E0r is the reflected amplitude and E0t the transmitted amplitude. Then the Fresnel equations are: rk = tk =

tan(θi − θt ) sin(θt − θi ) , r⊥ = tan(θi + θt ) sin(θt + θi )

2 sin(θt ) cos(θi ) 2 sin(θt ) cos(θi ) , t⊥ = sin(θt + θi ) cos(θt − θi ) sin(θt + θi )

The following holds: t⊥ − r⊥ = 1 and tk + rk = 1. If the coefficient of reflection R and transmission T are defined as (with θi = θr ): It cos(θt ) Ir and T ≡ R≡ Ii Ii cos(θi )

Chapter 6: Optics

27

~ it follows: R + T = 1. A special case is rk = 0. This happens if the angle between the reflected with I = h|S|i and transmitted rays is 90◦ . From Snell’s law it then follows: tan(θi ) = n. This angle is called Brewster’s angle. The situation with r⊥ = 0 is not possible.

6.6 Polarization The polarization is defined as: P =

Ip Imax − Imin = Ip + Iu Imax + Imin

where the intensity of the polarized light is given by Ip and the intensity of the unpolarized light is given by Iu . Imax and Imin are the maximum and minimum intensities when the light passes a polarizer. If polarized light passes through a polarizer Malus law applies: I(θ) = I(0) cos2 (θ) where θ is the angle of the polarizer. The state of a light ray can be described by the Stokes-parameters: start with 4 filters which each transmits half the intensity. The first is independent of the polarization, the second and third are linear polarizers with the transmission axes horizontal and at +45◦ , while the fourth is a circular polarizer which is opaque for L-states. Then holds S1 = 2I1 , S2 = 2I2 − 2I1 , S3 = 2I3 − 2I1 and S4 = 2I4 − 2I1 . The state of a polarized light ray can also be described by the Jones vector:   E0x eiϕx ~ E= E0y eiϕy ~ = (1, 0), for the vertical P -state E ~ = (0, 1), the R-state is given by For the √ horizontal P -state holds: E √ 1 1 ~ ~ E = 2 2(1, −i) and the L-state by E = 2 2(1, i). The change in state of a light beam after passage of ~ 1 . For some types of optical equipment the Jones matrix M ~2 = M · E optical equipment can be described as E is given by:   1 0 Horizontal linear polarizer: 0 0   0 0 Vertical linear polarizer: 0 1   1 1 1 ◦ Linear polarizer at +45 2 1 1   1 −1 1 Lineair polarizer at −45◦ 2 −1 1   1 0 1 iπ/4 -λ plate, fast axis vertical e 4 0 −i   1 0 1 iπ/4 e 4 -λ plate, fast axis horizontal 0 i   1 i 1 Homogene circular polarizor right 2 −i 1   1 −i 1 Homogene circular polarizer left 2 i 1

6.7 Prisms and dispersion A light ray passing through a prism is refracted twice and aquires a deviation from its original direction δ = θi + θi0 + α w.r.t. the incident direction, where α is the apex angle, θi is the angle between the incident angle and a line perpendicular to the surface and θi0 is the angle between the ray leaving the prism and a line perpendicular to the surface. When θi varies there is an angle for which δ becomes minimal. For the refractive index of the prism now holds: sin( 12 (δmin + α)) n= sin( 12 α)

Physics Formulary by ir. J.C.A. Wevers

28

The dispersion of a prism is defined by: dδ dn dδ = dλ dn dλ where the first factor depends on the shape and the second on the composition of the prism. For the first factor follows: 2 sin( 12 α) dδ = dn cos( 12 (δmin + α)) D=

For visible light usually holds dn/dλ < 0: shorter wavelengths are stronger bent than longer. The refractive index in this area can usually be approximated by Cauchy’s formula.

6.8 Diffraction Fraunhofer diffraction occurs far away from the source(s). The Fraunhofer diffraction of light passing through multiple slits is described by:  2  2 sin(u) sin(N v) I(θ) = · I0 u sin(v) where u = πb sin(θ)/λ, v = πd sin(θ)/λ. N is the number of slits, b the width of a slit and d the distance between the slits. The maxima in intensity are given by d sin(θ) = kλ. The diffraction through a spherical aperture with radius a is described by: I(θ) = I0



J1 (ka sin(θ)) ka sin(θ)

2

The diffraction pattern of a rectangular aperture at distance R with length a in the x-direction and b in the y-direction is described by:  2  2 sin(α0 ) sin(β 0 ) I(x, y) = I0 α0 β0 where α0 = kax/2R and β 0 = kby/2R. When X rays are diffracted at a crystal holds for the position of the maxima in intensity Bragg’s relation: 2d sin(θ) = nλ where d is the distance between the crystal layers. Close at the source the Fraunhofermodel is invalid because it ignores the angle-dependence of the reflected waves. This is described by the obliquity or inclination factor, which describes the directionality of the secondary emissions: E(θ) = 12 E0 (1 + cos(θ)) where θ is the angle w.r.t. the optical axis. Diffraction limits the resolution of a system. This is the minimum angle ∆θmin between two incident rays coming from points far away for which their refraction patterns can be detected separately. For a circular slit holds: ∆θmin = 1.22λ/D where D is the diameter of the slit. For a grating holds: ∆θmin = 2λ/(N a cos(θm )) where a is the distance between two peaks and N the number of peaks. The minimum difference between two wavelengths that gives a separated diffraction pattern in a multiple slit geometry is given by ∆λ/λ = nN where N is the number of lines and n the order of the pattern.

6.9 Special optical effects ~ is not parallel with E ~ if the polarizability P~ of a material is not equal in • Birefringe and dichroism. D all directions. There are at least 3 directions, the principal axes, in which they are parallel. This results in 3 refractive indices ni which can be used to construct Fresnel’s ellipsoid. In case n2 = n3 6= n1 , which happens e.g. at trigonal, hexagonal and tetragonal crystals there is one optical axis in the direction of n1 . Incident light rays can now be split up in two parts: the ordinary wave is linear polarized ⊥ the plane through the transmission direction and the optical axis. The extraordinary wave is linear polarized

Chapter 6: Optics

29

in the plane through the transmission direction and the optical axis. Dichroism is caused by a different absorption of the ordinary and extraordinary wave in some materials. Double images occur when the incident ray makes an angle with the optical axis: the extraordinary wave will refract, the ordinary will not. • Retarders: waveplates and compensators. Incident light will have a phase shift of ∆ϕ = 2πd(|n0 − ne |)/λ0 if an uniaxial crystal is cut in such a way that the optical axis is parallel with the front and back plane. Here, λ0 is the wavelength in vacuum and n0 and ne the refractive indices for the ordinary and extraordinary wave. For a quarter-wave plate holds: ∆ϕ = π/2. • The Kerr-effect: isotropic, transparent materials can become birefringent when placed in an electric ~ The difference in refractive index in the two directions field. In that case, the optical axis is parallel to E. is given by: ∆n = λ0 KE 2 , where K is the Kerr constant of the material. If the electrodes have an effective length ` and are separated by a distance d, the retardation is given by: ∆ϕ = 2πK`V 2 /d2 , where V is the applied voltage. • The Pockels or linear electro-optical effect can occur in 20 (from a total of 32) crystal symmetry classes, namely those without a centre of symmetry. These crystals are also piezoelectric: their polarization ~ The retardation in a Pockels cell is changes when a pressure is applied and vice versa: P~ = pd + ε0 χE. 3 ∆ϕ = 2πn0 r63 V /λ0 where r63 is the 6-3 element of the electro-optic tensor. • The Faraday effect: the polarization of light passing through material with length d and to which a magnetic field is applied in the propagation direction is rotated by an angle β = VBd where V is the Verdet constant. ˘ • Cerenkov radiation arises when a charged particle with vq > vf arrives. The radiation is emitted within a cone with an apex angle α with sin(α) = c/cmedium = c/nvq .

6.10 The Fabry-Perot interferometer For a Fabry-Perot interferometer holds in general: T + R + A = 1 where T is the transmission factor, R the reflection factor and A the absorption factor. If F is given by F = 4R/(1 − R)2 it follows for the intensity distribution:  2 A 1 It = 1− Ii 1 − R 1 + F sin2 (θ) The term [1 + F sin2 (θ)]−1 := A(θ) is called the Airy function.

PP PP q d

Screen Focussing lens √ √ The width of the peaks at half height is given by γ = 4/ F . The finesse F is defined as F = 12 π F . The maximum resolution is then given by ∆fmin = c/2ndF. Source

Lens

Chapter 7

Statistical physics 7.1 Degrees of freedom A molecule consisting of n atoms has s = 3n degrees of freedom. There are 3 translational degrees of freedom, a linear molecule has s = 3n − 5 vibrational degrees of freedom and a non-linear molecule s = 3n − 6. A linear molecule has 2 rotational degrees of freedom and a non-linear molecule 3. Because vibrational degrees of freedom account for both kinetic and potential energy they count double. So, for linear molecules this results in a total of s = 6n − 5. For non-linear molecules this gives s = 6n − 6. The average energy of a molecule in thermodynamic equilibrium is hEtot i = 12 skT . Each degree of freedom of a molecule has in principle the same energy: the principle of equipartition. The rotational and vibrational energy of a molecule are: Wrot =

¯2 h l(l + 1) = Bl(l + 1) , Wvib = (v + 12 )¯hω0 2I

The vibrational levels are excited if kT ≈ ¯hω, the rotational levels of a hetronuclear molecule are excited if kT ≈ 2B. For homonuclear molecules additional selection rules apply so the rotational levels are well coupled if kT ≈ 6B.

7.2 The energy distribution function The general form of the equilibrium velocity distribution function is P (vx , vy , vz )dvx dvy dvz = P (vx )dvx · P (vy )dvy · P (vz )dvz with  2 v 1 P (vi )dvi = √ exp − i2 dvi α α π p where α =

2kT  /m is the most probable velocity of a particle. The average velocity is given by hvi = √ 2α/ π, and v 2 = 32 α2 . The distribution as a function of the absolute value of the velocity is given by:   4N mv 2 dN = 3 √ v 2 exp − dv α π 2kT The general form of the energy distribution function then becomes: P (E)dE =

c(s) kT



E kT

 12 s−1

where c(s) is a normalization constant, given by: 1. Even s: s = 2l: c(s) =

1 (l − 1)!

2. Odd s: s = 2l + 1: c(s) = √

2l π(2l − 1)!! 30

  E exp − dE kT

Chapter 7: Statistical physics

31

7.3 Pressure on a wall The number of molecules that collides with a wall with surface A within a time τ is given by: Z∞ Zπ Z2π

ZZZ 3

d N=

nAvτ cos(θ)P (v, θ, ϕ)dvdθdϕ 0

0

0

From this follows for the particle flux on the wall: Φ = 14 n hvi. For the pressure on the wall then follows: d3 p =

2 2mv cos(θ)d3 N , so p = n hEi Aτ 3

7.4 The equation of state If intermolecular forces and the volume of the molecules can be neglected then for gases from p = and hEi = 32 kT can be derived:

 1 pV = ns RT = N m v 2 3

2 3 n hEi

Here, ns is the number of moles particles and N is the total number of particles within volume V . If the own volume and the intermolecular forces cannot be neglected the Van der Waals equation can be derived:   an2 p + 2s (V − bns ) = ns RT V There is an isotherme with a horizontal point of inflection. In the Van der Waals equation this corresponds with the critical temperature, pressure and volume of the gas. This is the upper limit of the area of coexistence between liquid and vapor. From dp/dV = 0 and d2 p/dV 2 = 0 follows: Tcr =

8a a , pcr = , Vcr = 3bns 27bR 27b2

For the critical point holds: pcr Vm,cr /RTcr = general gas law.

3 8,

which differs from the value of 1 which follows from the

Scaled on the critical quantities, with p∗ := p/pcr , T ∗ = T /Tcr and Vm∗ = Vm /Vm,cr with Vm := V /ns holds:  p∗ +



3 (Vm∗ )2

Vm∗ −

1 3




= 83 T ∗

Gases behave the same for equal values of the reduced quantities: the law of the corresponding states. A virial expansion is used for even more accurate views:  p(T, Vm ) = RT

 1 B(T ) C(T ) + + + · · · Vm Vm2 Vm3

The Boyle temperature TB is the temperature for which the 2nd virial coefficient is 0. In a Van der Waals gas, this happens at TB = a/Rb. The inversion temperature Ti = 2TB . The equation of state for solids and liquids is given by: 1 V = 1 + γp ∆T − κT ∆p = 1 + V0 V



∂V ∂T

 ∆T + p

1 V



∂V ∂p

 ∆p T

Physics Formulary by ir. J.C.A. Wevers

32

7.5 Collisions between molecules The collision probability of a particle in a gas that is translated over a distance dx is given by nσdx, where σ is p v1 with u = v12 + v22 the relative velocity between the cross section. The mean free path is given by ` = nuσ r u m1 1 1 √ . This means . If m1 = m2 holds: ` = = 1+ , so ` = the particles. If m1  m2 holds: v1 m2 nσ nσ 2 1 . If the molecules are approximated by hard that the average time between two collisions is given by τ = nσv 1 2 2 spheres the cross section is: σ = 4 π(D1 + D2 ). The average distance between two molecules is 0.55n−1/3. Collisions between molecules and small particles in 

result  in the Brownian motion. For the average

a solution motion of a particle with radius R can be derived: x2i = 13 r2 = kT t/3πηR. A gas is called a Knudsen gas if `  the dimensions of the gas, something that can easily occur at low pressures. condition for a vessel which has a hole with surface A holds that p The equilibrium √ in it for which √ √ √ `  A/π is: n1 T1 = n2 T2 . Together with the general gas law follows: p1 / T1 = p2 / T2 . Awx . d The velocity profile between the plates is in that case given by w(z) = zwx /d. It can be derived that η = 1 3 %` hvi where v is the thermal velocity.   T2 − T1 dQ = κA , which results in a temperThe heat conductance in a non-moving gas is described by: dt d ature profile T (z) = T1 + z(T2 − T1 )/d. It can be derived that κ = 13 CmV n` hvi /NA . Also holds: κ = CV η. A better expression for κ can be obtained with the Eucken correction: κ = (1 + 9R/4cmV )CV · η with an error <5%. If two plates move along each other at a distance d with velocity wx the viscosity η is given by: Fx = η

7.6 Interaction between molecules For dipole interaction between molecules can be derived that U ∼ −1/r6 . If the distance between two molecules approaches the molecular diameter D a repulsing force between the electron clouds appears. This force can be described by Urep ∼ exp(−γr) or Vrep = +Cs /rs with 12 ≤ s ≤ 20. This results in the Lennard-Jones potential for intermolecular forces: "   6 # 12 D D − ULJ = 4 r r with a minimum  at r = rm . The following holds: D ≈ 0.89rm . For the Van der Waals coefficients a and b and the critical quantities holds: a = 5.275NA2 D3 , b = 1.3NA D3 , kTkr = 1.2 and Vm,kr = 3.9NA D3 . A more simple model for intermolecular forces assumes a potential U (r) = ∞ for r < D, U (r) = ULJ for D ≤ r ≤ 3D and U (r) = 0 for r ≥ 3D. This gives for the potential energy of one molecule: Epot = Z 3D U (r)F (r)dr. D

with F (r) the spatial distribution function in spherical coordinates, which for a homogeneous distribution is given by: F (r)dr = 4nπr2 dr. Some useful mathematical relations are: Z∞

n −x

x e 0

Z∞ dx = n! ,

2n −x2

x e 0

√ Z∞ 2 (2n)! π dx = , x2n+1 e−x dx = 12 n! n!22n+1 0

Chapter 8

Thermodynamics 8.1 Mathematical introduction If there exists a relation f (x, y, z) = 0 between 3 variables, one can write: x = x(y, z), y = y(x, z) and z = z(x, y). The total differential dz of z is than given by:     ∂z ∂z dx + dy dz = ∂x y ∂y x By writing this also for dx and dy it can be obtained that       ∂y ∂z ∂x · · = −1 ∂y z ∂z x ∂x y Because dz is a total differential holds

H

dz = 0.

A homogeneous function of degree m obeys: εm F (x, y, z) = F (εx, εy, εz). For such a function Euler’s theorem applies: ∂F ∂F ∂F +y +z mF (x, y, z) = x ∂x ∂y ∂z

8.2 Definitions 1 • The isochoric pressure coefficient: βV = p

 

∂p ∂T

 V



1 ∂V V ∂p T   1 ∂V • The isobaric volume coefficient: γp = V ∂T p   1 ∂V • The adiabatic compressibility: κS = − V ∂p S • The isothermal compressibility: κT = −

For an ideal gas follows: γp = 1/T , κT = 1/p and βV = −1/V .

8.3 Thermal heat capacity 

 ∂S ∂T X   ∂H • The specific heat at constant pressure: Cp = ∂T p   ∂U • The specific heat at constant volume: CV = ∂T V • The specific heat at constant X is: CX = T

33

Physics Formulary by ir. J.C.A. Wevers

34

For an ideal gas holds: Cmp − CmV = R. Further, if the temperature is high enough to thermalize all internal rotational and vibrational degrees of freedom, holds: CV = 12 sR. Hence Cp = 12 (s + 2)R. For their ratio now follows γ = (2 + s)/s. For a lower T one needs only to consider the thermalized degrees of freedom. For a Van der Waals gas holds: CmV = 12 sR + ap/RT 2. In general holds:

 Cp − CV = T

∂p ∂T



 · V

∂V ∂T



 = −T p

∂V ∂T

2  p

∂p ∂V

 ≥0 T

Because (∂p/∂V )T is always < 0, the following is always valid: Cp ≥ CV . If the coefficient of expansion is 0, Cp = CV , and also at T = 0K.

8.4 The laws of thermodynamics The zeroth law states that heat flows from higher to lower temperatures. The first law is the conservation of energy. For a closed system holds: Q = ∆U + W , where Q is the total added heat, W the work done and ∆U the difference in the internal energy. In differential form this becomes: d Q = dU + d W , where d means that the it is not a differential of a quantity of state. For a quasi-static process holds: d W = pdV . So for a reversible process holds: d Q = dU + pdV . For an open (flowing) system the first law is: Q = ∆H + Wi + ∆Ekin + ∆Epot . One can extract an amount of work Wt from the system or add Wt = −Wi to the system. The second law states: for a closed system there exists an additive quantity S, called the entropy, the differential of which has the following property: dQ dS ≥ T If the only processes occurring are reversible holds: dS = d Qrev /T . So, the entropy difference after a reversible process is: Z2 d Qrev S2 − S1 = T I So, for a reversible cycle holds: I For an irreversible cycle holds:

1

d Qrev = 0. T d Qirr < 0. T

The third law of thermodynamics is (Nernst):  lim

T →0

∂S ∂X

 =0 T

From this it can be concluded that the thermal heat capacity → 0 if T → 0, so absolute zero temperature cannot be reached by cooling through a finite number of steps.

8.5 State functions and Maxwell relations The quantities of state and their differentials are: Internal energy: Enthalpy: Free energy: Gibbs free enthalpy:

U H = U + pV F = U − TS G = H − TS

dU = T dS − pdV dH = T dS + V dp dF = −SdT − pdV dG = −SdT + V dp

Chapter 8: Thermodynamics

35

From this one can derive Maxwell’s relations:                 ∂p ∂T ∂V ∂p ∂S ∂V ∂S ∂T =− , = , = , =− ∂V S ∂S V ∂p S ∂S p ∂T V ∂V T ∂T p ∂p T From the total differential and the definitions of CV and Cp it can be derived that:     ∂p ∂V dV and T dS = Cp dT − T dp T dS = CV dT + T ∂T V ∂T p For an ideal gas also holds:         T T V p 0 + R ln + Sm0 and Sm = Cp ln − R ln + Sm0 Sm = CV ln T0 V0 T0 p0 Helmholtz’ equations are: 

∂U ∂V



 =T T

∂p ∂T



 −p , V

∂H ∂p



 =V −T T

∂V ∂T

 p

for an enlarged surface holds: d Wrev = −γdA, with γ the surface tension. From this follows:     ∂F ∂U = γ= ∂A S ∂A T

8.6 Processes The efficiency η of a process is given by: η =

Work done Heat added

The Cold factor ξ of a cooling down process is given by: ξ =

Cold delivered Work added

Reversible adiabatic processes For adiabatic processes holds: W = U1 − U2 . For reversible adiabatic processes holds Poisson’s equation: with γ = Cp /CV one gets that pV γ =constant. Also holds: T V γ−1 =constant and T γ p1−γ =constant. Adiabatics exhibit a greater steepness p-V diagram than isothermics because γ > 1. Isobaric processes Here holds: H2 − H1 =

R2 1

Cp dT . For a reversible isobaric process holds: H2 − H1 = Qrev .

The throttle process This is also called the Joule-Kelvin effect and is an adiabatic expansion of a gas through a porous material or a small opening. Here H is a conserved quantity, and dS > 0. In general this is accompanied with a change in temperature. The quantity which is important here is the throttle coefficient: # "     ∂T ∂V 1 = −V T αH = ∂p H Cp ∂T p The inversion temperature is the temperature where an adiabatically expanding gas keeps the same temperature. If T > Ti the gas heats up, if T < Ti the gas cools down. Ti = 2TB , with for TB : [∂(pV )/∂p]T = 0. The throttle process is e.g. applied in refridgerators. The Carnotprocess The system undergoes a reversible cycle with 2 isothemics and 2 adiabatics: 1. Isothermic expansion at T1 . The system absorbs a heat Q1 from the reservoir. 2. Adiabatic expansion with a temperature drop to T2 .

Physics Formulary by ir. J.C.A. Wevers

36

3. Isothermic compression at T2 , removing Q2 from the system. 4. Adiabatic compression to T1 . The efficiency for Carnot’s process is: η =1−

T2 |Q2 | =1− := ηC |Q1 | T1

The Carnot efficiency ηC is the maximal efficiency at which a heat machine can operate. If the process is applied in reverse order and the system performs a work −W the cold factor is given by: ξ=

|Q2 | T2 |Q2 | = = W |Q1 | − |Q2 | T1 − T2

The Stirling process Stirling’s cycle exists of 2 isothermics and 2 isochorics. The efficiency in the ideal case is the same as for Carnot’s cycle.

8.7 Maximal work Consider a system that changes from state 1 into state 2, with the temperature and pressure of the surroundings given by T0 and p0 . The maximum work which can be obtained from this change is, when all processes are reversible: 1. Closed system: Wmax = (U1 − U2 ) − T0 (S1 − S2 ) + p0 (V1 − V2 ). 2. Open system: Wmax = (H1 − H2 ) − T0 (S1 − S2 ) − ∆Ekin − ∆Epot . The minimal work needed to attain a certain state is: Wmin = −Wmax .

8.8 Phase transitions Phase transitions are isothermic and isobaric, so dG = 0. When the phases are indicated by α, β and γ holds: β Gα m = Gm and rβα α β − Sm = ∆Sm = Sm T0 where rβα is the transition heat of phase β to phase α and T0 is the transition temperature. The following holds: rβα = rαβ and rβα = rγα − rγβ . Further   ∂Gm Sm = ∂T p so G has a twist in the transition point. In a two phase system Clapeyron’s equation is valid: β S α − Sm rβα dp = m = β α α dT Vm − Vm (Vm − Vmβ )T

For an ideal gas one finds for the vapor line at some distance from the critical point: p = p0 e−rβα/RT There exist also phase transitions with rβα = 0. For those there will occur only a discontinuity in the second derivates of Gm . These second-order transitions appear at organization phenomena. A phase-change of the 3rd order, so with e.g. [∂ 3 Gm /∂T 3 ]p non continuous arises e.g. when ferromagnetic iron changes to the paramagnetic state.

Chapter 8: Thermodynamics

37

8.9 Thermodynamic potential When the number of particles within a system changes this number becomes a third quantity of state. Because addition of matter usually takes place at constant p and T , G is the relevant quantity. If a system exists of more components this becomes: X µi dni dG = −SdT + V dp +  where µ =

∂G ∂ni

i



is called the thermodynamic potential. This is a partial quantity. For V holds: p,T,nj

V =

c X

 ni

i=1

∂V ∂ni

 := nj ,p,T

c X

ni Vi

i=1

where Vi is the partial volume of component i. The following holds: X xi Vi Vm = i

0

=

X

xi dVi

i

where xi = ni /n is the molar fraction of component i. The molar volume of a mixture of two components can be a concave line in a V -x2 diagram: the mixing contracts the volume. The system. It can be derived that P P thermodynamic potentials are not independent in a multiple-phase ni dµi = −SdT + V dp, this gives at constant p and T : xi dµi = 0 (Gibbs-Duhmen). i

i

Each component has as much µ’s as there are phases. The number of free parameters in a system with c components and p different phases is given by f = c + 2 − p.

8.10 Ideal mixtures For a mixture of n components holds (the index 0 is the value for the pure component): X X X ni Ui0 , Hmixture = ni Hi0 , Smixture = n xi Si0 + ∆Smix Umixture = i

where for ideal gases holds: ∆Smix = −nR

P

i

i

xi ln(xi ).

i

For the thermodynamic potentials holds: µi = µ0i + RT ln(xi ) < µ0i . A mixture of two liquids is rarely ideal: this is usually only the case for chemically related components or isotopes. In spite of this holds Raoult’s law for the vapour pressure holds for many binary mixtures: pi = xi p0i = yi p. Here is xi the fraction of the ith component in liquid phase and yi the fraction of the ith component in gas phase. A solution of one component in another gives rise to an increase in the boiling point ∆Tk and a decrease of the freezing point ∆Ts . For x2  1 holds: ∆Tk =

RTk2 RT 2 x2 , ∆Ts = − s x2 rβα rγβ

with rβα the evaporation heat and rγβ < 0 the melting heat. For the osmotic pressure Π of a solution holds: 0 = x2 RT . ΠVm1

8.11 Conditions for equilibrium When a system evolves towards equilibrium the only changes that are possible are those for which holds: (dS)U,V ≥ 0 or (dU )S,V ≤ 0 or (dH)S,p ≤ 0 or (dF )T,V ≤ 0 or (dG)T,p ≤ 0. In equilibrium for each β γ component holds: µα i = µi = µi .

Physics Formulary by ir. J.C.A. Wevers

38

8.12 Statistical basis for thermodynamics The number of possibilities P to distribute N particles on n possible energy levels, each with a g-fold degeneracy is called the thermodynamic probability and is given by: P = N!

Y g ni i

i

ni !

The most probable distribution, that with the maximum value for P , is the equilibrium state. When Stirling’s equation, ln(n!) ≈ n ln(n) − n is used, one finds for a discrete system the Maxwell-Boltzmann distribution. The occupation numbers in equilibrium are then given by:   N Wi ni = gi exp − Z kT P gi exp(−Wi /kT ). For an ideal gas holds: The state sum Z is a normalization constant, given by: Z = i

Z=

V (2πmkT )3/2 h3

The entropy can then be defined as: S = k ln(P ) . For a system in thermodynamic equilibrium this becomes: S=

U + kN ln T



Z N

 + kN ≈

U + k ln T 

For an ideal gas, with U = 32 kT then holds: S = 52 kN + kN ln



ZN N!



V (2πmkT )3/2 N h3



8.13 Application to other systems Thermodynamics can be applied to other systems than gases and liquids. To do this the term d W = pdV has to be replaced with the correct work term, like d Wrev = −F dl for the stretching of a wire, d Wrev = −γdA for the expansion of a soap bubble or d Wrev = −BdM for a magnetic system. hκ A rotating, non-charged black hole has a temparature of T = ¯hc/8πkm. It has an entropy S = Akc3 /4¯ with A the area of its event horizon. For a Schwarzschild black hole A is given by A = 16πm2 . Hawkings area theorem states that dA/dt ≥ 0. Hence, the lifetime of a black hole ∼ m3 .

Chapter 9

Transport phenomena 9.1 Mathematical introduction An important relation is: if X is a quantity of a volume element which travels from position ~r to ~r + d~r in a time dt, the total differential dX is then given by: dX =

∂X ∂X ∂X dX ∂X ∂X ∂X ∂X ∂X dx + dy + dz + dt ⇒ = vx + vy + vz + ∂x ∂y ∂z ∂t dt ∂x ∂y ∂z ∂t

∂X dX = + (~v · ∇)X . dt ∂t ZZZ ZZZ ZZ ∂ d Xd3 V = Xd3 V + X(~v · ~n )d2 A From this follows that also holds: dt ∂t

This results in general to:

where the volume V is surrounded by surface A. Some properties of the ∇ operator are: div(φ~v ) = φdiv~v + gradφ · ~v div(~u × ~v ) = ~v · (rot~u ) − ~u · (rot~v ) div gradφ = ∇2 φ

rot(φ~v ) = φrot~v + (gradφ) × ~v rot rot~v = grad div~v − ∇2~v ∇2~v ≡ (∇2 v1 , ∇2 v2 , ∇2 v3 )

rot gradφ = ~0 div rot~v = 0

Here, ~v is an arbitrary vector field and φ an arbitrary scalar field. Some important integral theorems are: ZZZ ZZ 2 (div~v )d3 V Gauss:

(~v · ~n )d A = ZZ

I

ZZ

I Stokes for a vector field:

(~n × gradφ)d2 A

(φ · ~et )ds =

Stokes for a scalar field:

(rot~v · ~n )d2 A

(~v · ~et )ds =

This results in:

ZZ

(rot~v · ~n )d2 A = 0

Ostrogradsky:

ZZZ ZZ 2 (rot~v )d3 A

(~n × ~v )d A = ZZZ ZZ 2 (gradφ)d3 V

(φ~n )d A =

Here, the orientable surface

RR

d2 A is limited by the Jordan curve

H

ds.

9.2 Conservation laws On a volume work two types of forces: 1. The force f~0 on each volume element. For gravity holds: f~0 = %~g. 2. Surface forces working only on the margins: ~t. For these holds: ~t = ~n T, where T is the stress tensor. 39

Physics Formulary by ir. J.C.A. Wevers

40

T can be split in a part pI representing the normal tensions and a part T0 representing the shear stresses: T = T0 + pI, where I is the unit tensor. When viscous aspects can be ignored holds: divT= −gradp. When the flow velocity is ~v at position ~r holds on position ~r + d~r: ~v (d~r ) =

~v (~r ) |{z}

+

translation

d~r · (grad~v ) {z } | rotation, deformation, dilatation

The quantity L:=grad~v can be split in a symmetric part D and an antisymmetric part W. L = D + W with     1 ∂vi ∂vj 1 ∂vi ∂vj + − , Wij := Dij := 2 ∂xj ∂xi 2 ∂xj ∂xi ~ represents the local rotation When the rotation or vorticity ~ ω = rot~v is introduced holds: Wij = 12 εijk ωk . ω 1 ~ ~ velocity: dr · W = 2 ω × dr. For a Newtonian liquid holds: T0 = 2ηD. Here, η is the dynamical viscosity. This is related to the shear stress τ by: ∂vi τij = η ∂xj For compressible media can be stated: T0 = (η 0 div~v )I + 2ηD. From equating the thermodynamical and mechanical pressure it follows: 3η 0 + 2η = 0. If the viscosity is constant holds: div(2D) = ∇2~v + grad div~v . The conservation laws for mass, momentum and energy for continuous media can be written in both integral and differential form. They are:

Integral notation: ∂ 1. Conservation of mass: ∂t

ZZZ

ZZ %d V + %(~v · ~n )d2 A = 0 3

ZZ ZZZ ZZ ZZZ ∂ 3 2 3 f0 d V + ~n · T d2 A %~v d V + %~v (~v · ~n )d A = 2. Conservation of momentum: ∂t ZZ ZZZ ∂ 3 1 2 ( 2 v + e)%d V + ( 12 v 2 + e)%(~v · ~n )d2 A = 3. Conservation of energy: ∂t ZZZ ZZ ZZ 2 3 ~ (~v · f0 )d V + (~v · ~n T)d2 A − (~ q · ~n )d A +

Differential notation: 1. Conservation of mass:

∂% + div · (%~v ) = 0 ∂t

2. Conservation of momentum: % 3. Conservation of energy: %T

∂~v + (%~v · ∇)~v = f~0 + divT = f~0 − gradp + divT0 ∂t

de p d% ds =% − = −div~q + T0 : D dt dt % dt

~ is Here, e is the internal energy per unit of mass E/m and s is the entropy per unit of mass S/m. ~q = −κ∇T the heat flow. Further holds: ∂e ∂E ∂e ∂E =− , T = = p=− ∂V ∂1/% ∂S ∂s so     ∂e ∂h and Cp = CV = ∂T V ∂T p with h = H/m the enthalpy per unit of mass.

Chapter 9: Transport phenomena

41

From this one can derive the Navier-Stokes equations for an incompressible, viscous and heat-conducting medium: div~v ∂~v + %(~v · ∇)~v % ∂t ∂T + %C(~v · ∇)T %C ∂t

=

0

=

%~g − gradp + η∇2~v

=

κ∇2 T + 2ηD : D

with C the thermal heat capacity. The force F~ on an object within a flow, when viscous effects are limited to the boundary layer, can be obtained using the momentum law. If a surface A surrounds the object outside the boundary layer holds: ZZ F~ = − [p~n + %~v (~v · ~n )]d2 A

9.3 Bernoulli’s equations Starting with the momentum equation one can find for a non-viscous medium for stationary flows, with (~v · grad)~v = 12 grad(v 2 ) + (rot~v ) × ~v and the potential equation ~g = −grad(gh) that: Z dp 1 2 = constant along a streamline 2 v + gh + % For compressible flows holds: 12 v 2 + gh + p/% =constant R along a line of flow. If also holds rot~v = 0 and the entropy is equal on each streamline holds 12 v 2 + gh + dp/% =constant everywhere. For incompressible flows this becomes: 12 v 2 + gh + p/% =constant everywhere. For ideal gases with constant Cp and CV holds, with γ = Cp /CV : γ p c2 1 2 1 2 2 v + γ − 1 % = 2 v + γ − 1 = constant With a velocity potential defined by ~v = gradφ holds for instationary flows: Z dp ∂φ 1 2 + 2 v + gh + = constant everywhere ∂t %

9.4 Characterising of flows by dimensionless numbers The advantage of dimensionless numbers is that they make model experiments possible: one has to make the dimensionless numbers which are important for the specific experiment equal for both model and the real situation. One can also deduce functional equalities without solving the differential equations. Some dimensionless numbers are given by: ωL v a Fo = ωL2 ν Pr = a

Strouhal: Sr = Fourier: Prandtl:

v2 gL vL P´eclet: Pe = a Lα Nusselt: Nu = κ Froude: Fr =

v c vL Reynolds: Re = ν v2 Eckert: Ec = c∆T Mach:

Ma =

Here, ν = η/% is the kinematic viscosity, c is the speed of sound and L is a characteristic length of the system. α follows from the equation for heat transport κ∂y T = α∆T and a = κ/%c is the thermal diffusion coefficient. These numbers can be interpreted as follows: • Re: (stationary inertial forces)/(viscous forces)

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• Sr: (non-stationary inertial forces)/(stationary inertial forces) • Fr: (stationary inertial forces)/(gravity) • Fo: (heat conductance)/(non-stationary change in enthalpy) • Pe: (convective heat transport)/(heat conductance) • Ec: (viscous dissipation)/(convective heat transport) • Ma: (velocity)/(speed of sound): objects moving faster than approximately Ma = 0,8 produce shockwaves which propagate with an angle θ with the velocity of the object. For this angle holds Ma= 1/ arctan(θ). • Pr and Nu are related to specific materials. Now, the dimensionless Navier-Stokes equation becomes, with x0 = x/L, ~v 0 = ~v /V , grad0 = Lgrad, ∇02 = L2 ∇2 and t0 = tω: ∇02~v 0 ~g ∂~v 0 + Sr 0 + (~v 0 · ∇0 )~v 0 = −grad0 p + ∂t Fr Re

9.5 Tube flows For tube flows holds: they are laminar if Re< 2300 with dimension of length the diameter of the tube, and turbulent if Re is larger. For an incompressible laminar flow through a straight, circular tube holds for the velocity profile: 1 dp 2 (R − r2 ) v(r) = − 4η dx ZR v(r)2πrdr = −

For the volume flow holds: ΦV =

π dp 4 R 8η dx

0

The entrance length Le is given by: 1. 500 < ReD < 2300: Le /2R = 0.056ReD 2. Re > 2300: Le /2R ≈ 50

√ 4R3 α π dp 3 dx 2 For flows at a small Re holds: ∇p = η∇ ~v and div~v = 0. For the total force on a sphere with radius R in a flow then holds: F = 6πηRv. For large Re holds for the force on a surface A: F = 12 CW A%v 2 . For gas transport at low pressures (Knudsen-gas) holds: ΦV =

9.6 Potential theory I The circulation Γ is defined as: Γ =

ZZ (~v · ~et )ds =

ZZ (rot~v ) · ~nd2 A =

(~ω · ~n )d2 A

For non viscous media, if p = p(%) and all forces are conservative, Kelvin’s theorem can be derived: dΓ =0 dt For rotationless flows a velocity potential ~v = gradφ can be introduced. In the incompressible case follows from conservation of mass ∇2 φ = 0. For a 2-dimensional flow a flow function ψ(x, y) can be defined: with ΦAB the amount of liquid flowing through a curve s between the points A and B: ΦAB

ZB ZB = (~v · ~n )ds = (vx dy − vy dx) A

A

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43

and the definitions vx = ∂ψ/∂y, vy = −∂ψ/∂x holds: ΦAB = ψ(B) − ψ(A). In general holds: ∂2ψ ∂2ψ + = −ωz 2 ∂x ∂y 2 In polar coordinates holds: ∂φ 1 ∂φ 1 ∂ψ ∂ψ = , vθ = − = r ∂θ ∂r ∂r r ∂θ Q ln(r) so that vr = Q/2πr, vθ = 0. For source flows with power Q in (x, y) = (0, 0) holds: φ = 2π vr =

For a dipole of strength Q in x = a and strength −Q in x = −a follows from superposition: φ = −Qax/2πr2 where Qa is the dipole strength. For a vortex holds: φ = Γθ/2π. If an object is surrounded by an uniform main flow with ~v = v~ex and such a large Re that viscous effects are limited to the boundary layer holds: Fx = 0 and Fy = −%Γv. The statement that Fx = 0 is d’Alembert’s paradox and originates from the neglection of viscous effects. The lift Fy is also created by η because Γ 6= 0 due to viscous effects. Henxe rotating bodies also create a force perpendicular to their direction of motion: the Magnus effect.

9.7 Boundary layers 9.7.1 Flow boundary layers

√ If for the thickness of the boundary layer holds: δ  L holds: δ ≈ L/ Re. With v∞ the velocity of the main flow it follows for the velocity vy ⊥ the surface: vy L ≈ δv∞ . Blasius’ equation for the boundary layer is, with vy /v∞ = f (y/δ): 2f 000 + f f 00 = 0 with boundary conditions f (0) = f 0 (0) = 0, f 0 (∞) = 1. From this follows: CW = 0.664 Rex−1/2 . The momentum theorem of Von Karman for the boundary layer is:

τ0 dv d (ϑv 2 ) + δ ∗ v = dx dx %

where the displacement thickness δ ∗ v and the momentum thickness ϑv 2 are given by: Z∞ Z∞ ∂vx ∗ ϑv = (v − vx )vx dy , δ v = (v − vx )dy and τ0 = −η ∂y 2

0

y=0

0

 The boundary layer is released from the surface if

∂vx ∂y

 = 0. This is equivalent with y=0

9.7.2 Temperature boundary layers

12ηv∞ dp = . dx δ2

√ If the thickness of the temperature boundary layer δT  L holds: 1. If Pr ≤ 1: δ/δT ≈ √Pr. 2. If Pr  1: δ/δT ≈ 3 Pr.

9.8 Heat conductance For non-stationairy heat conductance in one dimension without flow holds: κ ∂2T ∂T = +Φ ∂t %c ∂x2 where Φ is a source term. If Φ = 0 the solutions for harmonic oscillations at x = 0 are:   x x T − T∞ cos ωt − = exp − Tmax − T∞ D D

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p with D = 2κ/ω%c. At x = πD the temperature variation is in anti-phase with the surface. The onedimensional solution at Φ = 0 is   x2 1 exp − T (x, t) = √ 4at 2 πat This is mathematical equivalent to the diffusion problem: ∂n = D∇2 n + P − A ∂t where P is the production of and A the discharge of particles. The flow density J = −D∇n.

9.9 Turbulence √ The time scale of turbulent velocity variations τt is of the order of: τt = τ Re/Ma2 with τ the molecular time scale. For the velocity of the particles holds: v(t) = hvi + v 0 (t) with hv 0 (t)i = 0. The Navier-Stokes equation now becomes: ∇ hpi divSR ∂ h~v i + (h~v i · ∇) h~v i = − + ν∇2 h~v i + ∂t % %

 where SR ij = −% hvi vj i is the turbulent stress tensor. Boussinesq’s assumption is: τij = −% vi0 vj0 . It is stated that, analogous to Newtonian media: SR = 2%νt hDi. Near a boundary holds: νt = 0, far away of a boundary holds: νt ≈ νRe.

9.10 Self organization ∂ω dω = + J(ω, ψ) = ν∇2 ω dt ∂t With J(ω, ψ) the Jacobian. So if ν = 0, ω is conserved. Further, the kinetic energy/mA and the enstrofy V are conserved: with ~v = ∇ × (~kψ) For a (semi) two-dimensional flow holds:

Z∞ E ∼ (∇ψ) ∼

Z∞ E(k, t)dk = constant , V ∼ (∇ ψ) ∼

2

2

0

k 2 E(k, t)dk = constant

2

0

From this follows that in a two-dimensional flow the energy flux goes towards large values of k: larger structures become larger at the expanse of smaller ones. In three-dimensional flows the situation is just the opposite.

Chapter 10

Quantum physics 10.1 Introduction to quantum physics 10.1.1 Black body radiation Planck’s law for the energy distribution for the radiation of a black body is: w(f ) =

8πhc 1 1 8πhf 3 , w(λ) = 3 5 hf /kT hc/λkT c λ e e −1 −1

Stefan-Boltzmann’s law for the total power density can be derived from this: P = AσT 4 . Wien’s law for the maximum can also be derived from this: T λmax = kW .

10.1.2 The Compton effect For the wavelength of scattered light, if light is considered to exist of particles, can be derived: λ0 = λ +

h (1 − cos θ) = λ + λC (1 − cos θ) mc

10.1.3 Electron diffraction Diffraction of electrons at a crystal can be explained by assuming that particles have a wave character with wavelength λ = h/p. This wavelength is called the Broglie-wavelength.

10.2 Wave functions The wave character of particles is described by a wavefunction ψ. This wavefunction can be described in normal or momentum space. Both definitions are each others Fourier transform: Z Z 1 1 −ikx dx and Ψ(x, t) = √ Ψ(x, t)e Φ(k, t)eikx dk Φ(k, t) = √ h h ¯ ω. These waves define a particle with group velocity vg = p/m and energy E = h The wavefunction can be interpreted as a measure for the probability P to find a particle somewhere (Born): dP = |ψ|2 d3 V . The expectation value hf i of a quantity f of a system is given by: ZZZ ZZZ ∗ 3 Φ∗ f Φd3 Vp hf (t)i = Ψ f Ψd V , hfp (t)i = This is also written as hf (t)i = hΦ|f |Φi. The normalizing condition for wavefunctions follows from this: hΦ|Φi = hΨ|Ψi = 1.

10.3 Operators in quantum physics In quantum mechanics, classical quantities are translated into operators. These operators are hermitian because their eigenvalues must be real: Z Z ψ1∗ Aψ2 d3 V =

45

ψ2 (Aψ1 )∗ d3 V

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When un is the eigenfunction of P the eigenvalue equation AΨ = aΨ for eigenvalue an , Ψ can be expanded into cn un . If this basis is taken orthonormal, then follows for the coefficients: a basis of eigenfunctions: Ψ = n

cn = hun |Ψi. If the system is in a state described by Ψ, the chance to find eigenvalue an when measuring A is given by |cn |2 in the discrete part of the spectrum and |cn |2 da in the continuous part of the spectrum between a and P a + da. The matrix element P Aij is given by: Aij = hui |A|uj i. Because (AB)ij = hui |AB|uj i = |un ihun | = 1. hui |A |un i hun |B|uj i holds: n

n

The time-dependence of an operator is given by (Heisenberg): ∂A [A, H] dA = + dt ∂t i¯h with [A, B] ≡ AB − BA the commutator of A and B. For hermitian operators the commutator is always complex. If [A, B] = 0, the operators A and B have a common set of eigenfunctions. By applying this to px and x follows (Ehrenfest): md2 hxit /dt2 = − hdU (x)/dxi. The first order approximation hF (x)it ≈ F (hxi), with F = −dU/dx represents the classical equation. Before the addition of quantummechanical operators which are a product of other operators, they should be made symmetrical: a classical product AB becomes 12 (AB + BA).

10.4 The uncertainty principle

  2 If the uncertainty ∆A in A is defined as: (∆A)2 = ψ|Aop − hAi |2 ψ = A2 − hAi it follows: ∆A · ∆B ≥ 12 | hψ|[A, B]|ψi | ¯ , and because [x, px ] = i¯h holds: ∆px · ∆x ≥ 12 h ¯ , and ∆Lx · ∆Ly ≥ 12 h ¯ Lz . From this follows: ∆E · ∆t ≥ 12 h

10.5 The Schr¨odinger equation The momentum operator is given by: pop = −i¯h∇. The position operator is: xop = i¯h∇p . The energy h∂/∂t. The Hamiltonian of a particle with mass m, potential energy U and total operator is given by: Eop = i¯ energy E is given by: H = p2 /2m + U . From Hψ = Eψ then follows the Schr¨odinger equation: −

¯2 2 h ∂ψ ∇ ψ + U ψ = Eψ = i¯h 2m ∂t

The linear combination of the solutions of this equation give the general solution. In one dimension it is:   X Z  iEt ψ(x, t) = + dE c(E)uE (x) exp − ¯h h ¯ (ψ ∗ ∇ψ − ψ∇ψ ∗ ) 2im ∂P (x, t) = −∇J(x, t) The following conservation law holds: ∂t

The current density J is given by: J =

10.6 Parity The parity operator in one dimension is given by Pψ(x) = ψ(−x). If the wavefunction is split in even and odd functions, it can be expanded into eigenfunctions of P: ψ(x) = 12 (ψ(x) + ψ(−x)) + 12 (ψ(x) − ψ(−x)) | {z } | {z } + − even: ψ odd: ψ [P, H] = 0. The functions ψ + = 12 (1 + P)ψ(x, t) and ψ − = 12 (1 − P)ψ(x, t) both satisfy the Schr¨odinger equation. Hence, parity is a conserved quantity.

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47

10.7 The tunnel effect The wavefunction of a particle in an ∞ high potential step from x = 0 to x = a is given by ψ(x) = a−1/2 sin(kx). The energylevels are given by En = n2 h2 /8a2 m. If the wavefunction with energy W meets a potential well of W0 > W the wavefunction will, unlike the classical case, be non-zero within the potential well. If 1, 2 and 3 are the areas in front, within and behind the potential well, holds: 0

0

ψ1 = Aeikx + Be−ikx , ψ2 = Ceik x + De−ik x , ψ3 = A0 eikx with k 02 = 2m(W − W0 )/¯ h2 and k 2 = 2mW . Using the boundary conditions requiring continuity: ψ = continuous and ∂ψ/∂x =continuous at x = 0 and x = a gives B, C and D and A0 expressed in A. The amplitude T of the transmitted wave is defined by T = |A0 |2 /|A|2 . If W > W0 and 2a = nλ0 = 2πn/k 0 holds: T = 1.

10.8 The harmonic oscillator For a harmonic oscillator holds: U = 12 bx2 and ω02 = b/m. The Hamiltonian H is then given by: H= with

q A=

1 2 mωx

p2 + 1 mω 2 x2 = 12 h ¯ ω + ωA† A 2m 2 ip and A† = +√ 2mω

q

1 2 mωx

ip −√ 2mω

¯ and [A, H] = h ¯ ωA. A is a so called raising ladder operator, A† a A 6= A† is non hermitian. [A, A† ] = h hω)AuE . There is an eigenfunction u0 for which holds: Au0 = 0. lowering ladder operator. HAuE = (E − ¯ hω: the zero point energy. For the normalized eigenfunctions follows: The energy in this ground state is 12 ¯ 1 un = √ n!



A† √ h ¯

r

n u0 with u0 =

4

  mωx2 mω exp − π¯h 2¯ h

with En = ( 12 + n)¯hω.

10.9 Angular momentum For the angular momentum operators L holds: [Lz , L2 ] = [Lz , H] = [L2 , H] = 0. However, cyclically holds: hLz . Not all components of L can be known at the same time with arbitrary accuracy. For Lz [Lx , Ly ] = i¯ holds:   ∂ ∂ ∂ = −i¯h x −y Lz = −i¯h ∂ϕ ∂y ∂x The ladder operators L± are defined by: L± = Lx ± iLy . Now holds: L2 = L+ L− + L2z − ¯hLz . Further,   ∂ ∂ + i cot(θ) ¯ e±iϕ ± L± = h ∂θ ∂ϕ hL+ follows: Lz (L+ Ylm ) = (m + 1)¯ h(L+ Ylm ). From [L+ , Lz ] = −¯ ¯ L− follows: Lz (L− Ylm ) = (m − 1)¯h(L− Ylm ). From [L− , Lz ] = h h2 (L± Ylm ). From [L2 , L± ] = 0 follows: L2 (L± Ylm ) = l(l + 1)¯ Because Lx and Ly are hermitian (this implies L†± = L∓ ) and |L± Ylm |2 > 0 follows: l(l + 1) − m2 − m ≥ 0 ⇒ −l ≤ m ≤ l. Further follows that l has to be integral or half-integral. Half-odd integral values give no unique solution ψ and are therefore dismissed.

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10.10 Spin For the spin operators are defined by their commutation relations: [Sx , Sy ] = i¯hSz . Because the spin operators do not act in the physical space (x, y, z) the uniqueness of the wavefunction is not a criterium here: also half odd-integer values are allowed for the spin. Because [L, S] = 0 spin and angular momentum operators do not ~~ have a common set of eigenfunctions. The spin operators are given by S = 1 ¯h~~σ , with  ~ ~σ x =

0 1 1 0



 , ~~σ y =

0 −i i 0



 , ~~σ z =

2

1 0 0 −1



The eigenstates of Sz are called spinors: χ = α+ χ+ + α− χ− , where χ+ = (1, 0) represents the state with h) and χ− = (0, 1) represents the state with spin down (Sz = − 12 ¯h). Then the probability spin up (Sz = 12 ¯ to find spin up after a measurement is given by |α+ |2 and the chance to find spin down is given by |α− |2 . Of course holds |α+ |2 + |α− |2 = 1. ~ ~ due to its spin, given by M ~ = −egS S/2m, The electron will have an intrinsic magnetic dipole moment M with gS = 2(1 + α/2π + · · ·) the gyromagnetic ratio. In the presence of an external magnetic field this gives ~ · B. ~ The Schr¨odinger equation then becomes (because ∂χ/∂xi ≡ 0): a potential energy U = −M i¯ h

egS ¯h ∂χ(t) ~ = ~σ · Bχ(t) ∂t 4m

~σ y , ~ ~σ z ). If B ~ = B~ez there are two eigenvalues for this problem: χ± for E = ±egS ¯hB/4m = with ~σ = (~ ~σ x , ~ ±¯hω. So the general solution is given by χ = (ae−iωt , beiωt ). From this can be derived: hSx i = 12 ¯h cos(2ωt) h sin(2ωt). Thus the spin precesses about the z-axis with frequency 2ω. This causes the normal and hSy i = 12 ¯ Zeeman splitting of spectral lines. The potential operator for two particles with spin ± 12 ¯h is given by: V (r) = V1 (r) +

1 ~ ~ (S1 · S2 )V2 (r) = V1 (r) + 12 V2 (r)[S(S + 1) − 32 ] ¯2 h

This makes it possible for two states to exist: S = 1 (triplet) or S = 0 (Singlet).

10.11 The Dirac formalism If the operators for p and E are substituted in the relativistic equation E 2 = m20 c4 + p2 c2 , the Klein-Gordon equation is found:   1 ∂2 m20 c2 2 ∇ − 2 2− ψ(~x, t) = 0 c ∂t ¯h2 The operator 2 − m20 c2 /¯ h2 can be separated: 1 ∂2 m 2 c2 ∇ − 2 2 − 02 = c ∂t ¯ h 2



m 2 c2 ∂ γλ − 02 ∂xλ ¯ h

  m20 c2 ∂ + γµ ∂xµ ¯h2

where the Dirac matrices γ are given by: γλ γµ + γµ γλ = 2δλµ . From this it can be derived that the γ are hermitian 4 × 4 matrices given by:     0 −iσk I 0 , γ4 = γk = iσk 0 0 −I With this, the Dirac equation becomes:   m20 c2 ∂ + γλ ψ(~x, t) = 0 ∂xλ ¯h2 where ψ(x) = (ψ1 (x), ψ2 (x), ψ3 (x), ψ4 (x)) is a spinor.

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49

10.12 Atomic physics 10.12.1 Solutions The solutions of the Schr¨odinger equation in spherical coordinates if the potential energy is a function of r alone can be written as: ψ(r, θ, ϕ) = Rnl (r)Yl,ml (θ, ϕ)χms , with Clm Ylm = √ Plm (cos θ)eimϕ 2π For an atom or ion with one electron holds: Rlm (ρ) = Clm e−ρ/2 ρl L2l+1 n−l−1 (ρ) with ρ = 2rZ/na0 with a0 = ε0 h2 /πme e2 . The Lji are the associated Laguere functions and the Plm are the associated Legendre polynomials: |m|

Pl

(x) = (1 − x2 )m/2

 (−1)m n! −x −m dn−m −x n d|m|  2 l m e x − 1) (x) = (e x ) (x , L n (n − m)! dxn−m dx|m|

The parity of these solutions is (−1)l . The functions are 2

n−1 P

(2l + 1) = 2n2 -folded degenerated.

l=0

10.12.2 Eigenvalue equations The eigenvalue equations for an atom or ion with with one electron are: Equation

Eigenvalue

Range

Hop ψ = Eψ

En = µe4 Z 2 /8ε20 h2 n2

n≥1

Lzop Ylm = Lz Ylm

Lz = ml ¯h

−l ≤ ml ≤ l

L2op Ylm

2

= L Ylm

2

L = l(l + 1)¯ h

2

l
Szop χ = Sz χ

Sz = ms ¯h

ms = ± 12

2 Sop χ = S 2χ

S 2 = s(s + 1)¯ h2

s=

1 2

10.12.3 Spin-orbit interaction ~ +M ~ . The total magnetic dipole moment of an electron is then The total momentum is given by J~ = L ~ where gS = 2.0023 is the gyromagnetic ratio of the electron. ~ S = −(e/2me )(L ~ + gS S) ~ = M ~L + M M ~ ·S ~ = L2 + S 2 + 2Lz Sz + L+ S− + L− S+ . J has quantum numbers j Further holds: J 2 = L2 + S 2 + 2L 1 with possible values j = l ± 2 , with 2j + 1 possible z-components (mJ ∈ {−j, .., 0, .., j}). If the interaction ~ · L. ~ It can then be derived energy between S and L is small it can be stated that: E = En + ESL = En + aS that: |En |Z 2 α2 a= 2 ¯h nl(l + 1)(l + 12 ) After a relativistic correction this becomes: |En |Z 2 α2 E = En + n



3 1 − 4n j +

 1 2

The fine structure in atomic spectra arises from this. With gS = 2 follows for the average magnetic moment: ~ where g is the Land´e-factor: ~ av = −(e/2me )g¯ hJ, M g =1+

~ · J~ j(j + 1) + s(s + 1) − l(l + 1) S =1+ J2 2j(j + 1)

For atoms with more than one electron the following limiting situations occur:

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1. L − S coupling: for small atoms the electrostatic interaction is dominant and the state can be characterized by L, S, J, mJ . J ∈ {|L − S|, ..., L + S − 1, L + S} and mJ ∈ {−J, ..., J − 1, J}. The spectroscopic notation for this interaction is: 2S+1 LJ . 2S + 1 is the multiplicity of a multiplet. 2. j − j coupling: for larger atoms the electrostatic interaction is smaller than the Li · si interaction of an electron. The state is characterized by ji ...jn , J, mJ where only the ji of the not completely filled subshells are to be taken into account. The energy difference for larger atoms when placed in a magnetic field is: ∆E = gµB mJ B where g is the Land´e factor. For a transition between two singlet states the line splits in 3 parts, for ∆mJ = −1, 0 + 1. This results in the normal Zeeman effect. At higher S the line splits up in more parts: the anomalous Zeeman effect. Interaction with the spin of the nucleus gives the hyperfine structure.

10.12.4 Selection rules ~ · ~r |l1 m1 i|. Conservation of angular moFor the dipole transition matrix elements follows: p0 ∼ |hl2 m2 |E mentum demands that for the transition of an electron holds that ∆l = ±1. For an atom where L − S coupling is dominant further holds: ∆S = 0 (but not strict), ∆L = 0, ±1, ∆J = 0, ±1 except for J = 0 → J = 0 transitions, ∆mJ = 0, ±1, but ∆mJ = 0 is forbidden if ∆J = 0. For an atom where j − j coupling is dominant further holds: for the jumping electron holds, except ∆l = ±1, also: ∆j = 0, ±1, and for all other electrons: ∆j = 0. For the total atom holds: ∆J = 0, ±1 but no J = 0 → J = 0 transitions and ∆mJ = 0, ±1, but ∆mJ = 0 is forbidden if ∆J = 0.

10.13 Interaction with electromagnetic fields The Hamiltonian of an electron in an electromagnetic field is given by: H=

2 2 1 ~ 2 − eV = − ¯h ∇2 + e B ~ ·L ~ + e A2 − eV (~ p + eA) 2µ 2µ 2µ 2µ

where µ is the reduced mass of the system. The term ∼ A2 can usually be neglected, except for very strong ~ = B~ez it is given by e2 B 2 (x2 + y 2 )/8µ. fields or macroscopic motions. For B ~ − ∇f , V 0 = V + ∂f /∂t is applied to the potentials the wavefunction ~0 = A When a gauge transformation A 0 is also transformed according to ψ = ψeiqef /¯h with qe the charge of the particle. Because f = f (x, t), this is called a local gauge transformation, in contrast with a global gauge transformation which can always be applied.

10.14 Perturbation theory 10.14.1 Time-independent perturbation theory To solve the equation (H0 + λH1 )ψn = En ψn one has to find the eigenfunctions of H = H0 + λH1 . Suppose that φn is a complete set of eigenfunctions of the non-perturbed Hamiltonian H0 : H0 φn = En0 φn . Because φn is a complete set holds:     X cnk (λ)φk ψn = N (λ) φn +   k6=n

(1)

(2)

When cnk and En are being expanded into λ: cnk = λcnk + λ2 cnk + · · · (1) (2) En = En0 + λEn + λ2 En + · · ·

Chapter 10: Quantum physics

51

(1)

and this is put into the Schr¨odinger equation the result is: En = hφn |H1 |φn i and hφm |H1 |φn i if m 6= n. The second-order correction of the energy is then given by: c(1) nm = 0 En0 − Em X | hφk |H1 |φn i |2 X hφk |λH1 |φn i . So to first order holds: ψn = φn + φk . En(2) = 0 0 En − Ek En0 − Ek0 k6=n

k6=n

In case the levels are degenerated the above does not hold. In that case an orthonormal set eigenfunctions φni is chosen for each level n, so that hφmi |φnj i = δmn δij . Now ψ is expanded as:   X  X (1) X αi φni + λ cnk βi φki + · · · ψn = N (λ)   i

i

k6=n

(1)

0 0 + λEni is approximated by Eni := En0 . Substitution in the Schr¨odinger equation and taking dot Eni = Eni P P (1) αi hφnj |H1 |φni i = En αj . Normalization requires that |αi |2 = 1. product with φni gives: i

i

10.14.2 Time-dependent perturbation theory ∂ψ(t) = (H0 + λV (t))ψ(t) ∂t   X −iEn0 t (1) cn (t) exp φn with cn (t) = δnk + λcn (t) + · · · and the expansion ψ(t) = h ¯ n From the Schr¨odinger equation i¯ h

follows:

c(1) n (t)

λ = i¯ h

Zt

0

hφn |V (t )|φk i exp



i(En0 − Ek0 )t0 ¯h



dt0

0

10.15 N-particle systems 10.15.1 General Identical particles are indistinguishable. For the total wavefunction of a system of identical indistinguishable particles holds: 1. Particles with a half-odd integer spin (Fermions): ψtotal must be antisymmetric w.r.t. interchange of the coordinates (spatial and spin) of each pair of particles. The Pauli principle results from this: two Fermions cannot exist in an identical state because then ψtotal = 0. 2. Particles with an integer spin (Bosons): ψtotal must be symmetric w.r.t. interchange of the coordinates (spatial and spin) of each pair of particles. For a system of two electrons there are 2 possibilities for the spatial wavefunction. When a and b are the quantum numbers of electron 1 and 2 holds: ψS (1, 2) = ψa (1)ψb (2) + ψa (2)ψb (1) , ψA (1, 2) = ψa (1)ψb (2) − ψa (2)ψb (1) Because the particles do not approach each other closely the repulsion energy at ψA in this state is smaller. The following spin wavefunctions are possible: √ χA = 12 2[χ+ (1)χ− (2) − χ+ (2)χ− (1)] ms = 0  ms = +1  χ+ √(1)χ+ (2) 1 χS = 2[χ (1)χ (2) + χ (2)χ (1)] m + − + − s = 0  2 ms = −1 χ− (1)χ− (2) Because the total wavefunction must be antisymmetric it follows: ψtotal = ψS χA or ψtotal = ψA χS .

Physics Formulary by ir. J.C.A. Wevers

52

For N particles the symmetric spatial function is given by: X ψ(all permutations of 1..N ) ψS (1, ..., N ) = 1 The antisymmetric wavefunction is given by the determinant ψA (1, ..., N ) = √ |uEi (j)| N!

10.15.2 Molecules The wavefunctions of atom a and b are φa and φb . If the 2 atoms approach each other there are √ two possibilities: the total wavefunction approaches the bonding function with lower total energy ψB = 12 2(φa + φb ) or √ approaches the anti-bonding function with higher energy ψAB = 12 2(φa − φb ). If a molecular-orbital is symmetric w.r.t. the connecting axis, like a combination of two s-orbitals it is called a σ-orbital, otherwise a π-orbital, like the combination of two p-orbitals along two axes. The energy of a system is: E =

hψ|H|ψi . hψ|ψi

The energy calculated with this method is always higher than the real energy if ψ is only an approximation for the solutions of Hψ = Eψ. Also, if there are more functions to be chosen, P the function which gives the lowest energy is the best approximation. Applying this to the function ψ = ci φi one finds: (Hij − ESij )ci = 0. This equation has only solutions if the secular determinant |Hij − ESij | = 0. Here, Hij = hφi |H|φj i and Sij = hφi |φj i. αi := Hii is the Coulomb integral and βij := Hij the exchange integral. Sii = 1 and Sij is the overlap integral. The first approximation in the molecular-orbital theory is to place both electrons of a chemical bond in the bonding orbital: ψ(1, 2) = ψB (1)ψB (2). This results in a large electron density between the nuclei and therefore a repulsion. A better approximation is: ψ(1, 2) = C1 ψB (1)ψB (2) + C2 ψAB (1)ψAB (2), with C1 = 1 and C2 ≈ 0.6. In some atoms, such as C, it is energetical more suitable to form orbitals which are a linear combination of the s, p and d states. There are three ways of hybridization in C: √ 1. SP-hybridization: ψsp = 12 2(ψ2s ± ψ2pz ). There are 2 hybrid orbitals which are placed on one line under 180◦ . Further the 2px and 2py orbitals remain. p √ √ √ 2. SP2 hybridization: ψsp2 = ψ2s / 3 + c1 ψ2pz + c2 ψ2py , where (c1 , c2 ) ∈ {( 2/3, 0), (−1/ 6, 1/ 2) √ √ , (−1/ 6, −1/ 2)}. The 3 SP2 orbitals lay in one plane, with symmetry axes which are at an angle of 120◦ . 3. SP3 hybridization: ψsp3 = 12 (ψ2s ± ψ2pz ± ψ2py ± ψ2px ). The 4 SP3 orbitals form a tetraheder with the symmetry axes at an angle of 109◦280 .

10.16 Quantum statistics If a system exists in a state in which one has not the disposal of the maximal amount of information about the system, it can be described by a density matrix ρ. If thePprobability that the system is in state ψi is given by ai , ri hψi |A|ψi i. one can write for the expectation value a of A: hai = i

If ψ is expanded into an orthonormal basis {φk } as: ψ (i) = hAi =

X

P k

(i)

ck φk , holds:

(Aρ)kk = Tr(Aρ)

k

P ri |ψi ihψi |. The probability to find where ρlk = c∗k cl . ρ is hermitian, with Tr(ρ) = 1. Further holds ρ = eigenvalue an when measuring A is given by ρnn if one uses a basis of eigenvectors of A for {φk }. For the time-dependence holds (in the Schr¨odinger image operators are not explicitly time-dependent): i¯h

dρ = [H, ρ] dt

Chapter 10: Quantum physics

53

For a macroscopic system in equilibrium holds [H, ρ] = 0. If all quantumstates with the same energy are equally probable: Pi = P (Ei ), one can obtain the distribution: Pn (E) = ρnn =

X e−En /kT with the state sum Z = e−En /kT Z n

The thermodynamic quantities are related to these definitions as follows: F = −kT ln(Z), U = hHi = P P ∂ ln(Z), S = −k Pn ln(Pn ). For a mixed state of M orthonormal quantum states with pn En = − ∂kT n n probability 1/M follows: S = k ln(M ). The distribution function for the internal states for a system in thermal equilibrium is the most probable function. This function can be found by taking the maximum of theP function which gives P the number of states with Stirling’s equation: ln(n!) ≈ n ln(n) − n, and the conditions nk = N and nk Wk = W . For identical, k

k

indistinguishable particles which obey the Pauli exclusion principle the possible number of states is given by: P =

Y k

gk ! nk !(gk − nk )!

This results in the Fermi-Dirac statistics. For indistinguishable particles which do not obey the exclusion principle the possible number of states is given by: P = N!

Y g nk k

k

nk !

This results in the Bose-Einstein statistics. So the distribution functions which explain how particles are distributed over the different one-particle states k which are each gk -fold degenerate depend on the spin of the particles. They are given by: N gk 1. Fermi-Dirac statistics: integer spin. nk ∈ {0, 1}, nk = Zg exp((Ek − µ)/kT ) + 1 P gk ln[1 + exp((Ei − µ)/kT )]. with ln(Zg ) = N gk 2. Bose-Einstein statistics: half odd-integer spin. nk ∈ IN , nk = Zg exp((Ek − µ)/kT ) − 1 P with ln(Zg ) = − gk ln[1 − exp((Ei − µ)/kT )].

P Here, Zg is the large-canonical state sum and µ the chemical potential. It is found by demanding nk = N , and for it holds: lim µ = EF , the Fermi-energy. N is the total number of particles. The Maxwell-Boltzmann T →0

distribution can be derived from this in the limit Ek − µ  kT :     X Ek N Ek exp − gk exp − with Z = nk = Z kT kT k

With the Fermi-energy, the Fermi-Dirac and Bose-Einstein statistics can be written as: 1. Fermi-Dirac statistics: nk =

gk . exp((Ek − EF )/kT ) + 1

2. Bose-Einstein statistics: nk =

gk . exp((Ek − EF )/kT ) − 1

Chapter 11

Plasma physics 11.1 Introduction ne ne + n0 where ne is the electron density and n0 the density of the neutrals. If a plasma contains also negative charged ions α is not well defined. The degree of ionization α of a plasma is defined by: α =

The probability that a test particle collides with another is given by dP = nσdx where σ is the cross section. The collision frequency νc = 1/τc = nσv. The mean free path is given by λv = 1/nσ. The rate coefficient K is defined by K = hσvi. The number of collisions per unit of time and volume between particles of kind 1 and 2 is given by n1 n2 hσvi = Kn1 n2 . The potential of an electron is given by: s r   r ε0 kTe Ti ε0 kTe −e exp − ≈ with λD = V (r) = 4πε0 r λD e2 (ne Ti + ni Te ) ne e 2 because charge is shielded in a plasma. Here, λD is the Debye length. For distances < λD the plasma cannot be assumed to be quasi-neutral. Deviations of charge neutrality by thermic motion are compensated by oscillations with frequency s ne e 2 me ε 0

ωpe =

The distance of closest approximation when two equal charged particles collide for a deviation of π/2 is −1/3  λD  Lp . 2b0 = e2 /(4πε0 12 mv 2 ). A “neat” plasma is defined as a plasma for which holds: b0 < ne Here Lp := |ne /∇ne | is the gradient length of the plasma.

11.2 Transport Relaxation times are defined as τ = 1/νc . Starting with σm = 4πb20 ln(ΛC ) and with 12 mv 2 = kT it can be found that: √ √ 8 2πε20 m(kT )3/2 4πε20 m2 v 3 = τm = 4 ne ln(ΛC ) ne4 ln(ΛC ) For momentum transfer between electrons and ions holds for a Maxwellian velocity distribution: √ √ √ √ 6π 3ε20 me (kTe )3/2 6π 3ε20 mi (kTi )3/2 ≈ τei , τii = τee = ne e4 ln(ΛC ) ni e4 ln(ΛC ) The energy relaxation times for identical particles are equal to the momentum relaxation times. Because for e-i collisions the energy transfer is only ∼ 2me /mi this is a slow process. Approximately holds: τee : τei : p τie : τieE = 1 : 1 : mi /me : mi /me . The relaxation for e-o interaction is much more complicated. For T > 10 eV holds approximately: σeo = −2/5 , for lower energies this can be a factor 10 lower. 10−17 ve The resistivity η = E/J of a plasma is given by: √ e2 me ln(ΛC ) ne e 2 √ = η= me νei 6π 3ε20 (kTe )3/2 54

Chapter 11: Plasma physics

55

The diffusion coefficient D is defined by means of the flux Γ by ~Γ = n~vdiff = −D∇n. The equation of continuity is ∂t n + ∇(nvdiff ) = 0 ⇒ ∂t n = D∇2 n. One finds that D = 13 λv v. A rough estimate gives τD = Lp /D = L2p τc /λ2v . For magnetized plasma’s λv must be replaced with the cyclotron radius. In electrical ~ with µ = e/mνc the mobility of the particles. The Einstein ~ = e(ne µe + ni µi )E fields also holds J~ = neµE ratio is: kT D = µ e Because a plasma is electrically neutral electrons and ions are strongly coupled and they don’t diffuse independent. The coefficient of ambipolar diffusion Damb is defined by ~Γ = ~Γi = ~Γe = −Damb ∇ne,i . From this follows that kTe /e − kTi /e kTe µi ≈ Damb = 1/µe − 1/µi e In an external magnetic field B0 particles will move in spiral orbits with cyclotron radius ρ = mv/eB0 and with cyclotron frequency Ω = B0 e/m. The helical orbit is perturbed by collisions. A plasma is called magnetized if λv > ρe,i . So the electrons are magnetized if √ me e3 ne ln(ΛC ) ρe √ 2 = <1 λee 6π 3ε0 (kTe )3/2 B0 Magnetization of only the electrons is sufficient to confine the plasma reasonable because they are coupled ~ Combined with the to the ions by charge neutrality. In case of magnetic confinement holds: ∇p = J~ × B. two stationary Maxwell equations for the B-field these form the ideal magneto-hydrodynamic equations. For a uniform B-field holds: p = nkT = B 2 /2µ0 . ~ = If both magnetic and electric fields are present electrons and ions will move in the same direction. If E 2 ~ ~ ~ ~ ~ Er ~er + Ez ~ez and B = Bz ~ez the E × B drift results in a velocity ~u = (E × B )/B and the velocity in the r, ϕ plane is r(r, ˙ ϕ, t) = ~u + ρ ~˙ (t).

11.3 Elastic collisions 11.3.1 General The scattering angle of a particle in interaction with another particle, as shown in the figure at the right is: Z∞ s

χ = π − 2b ra

r2

1−

b @ I @ R

dr b2 W (r) − r2 E0

Particles with an impact parameter between b and b + db, moving through a ring with dσ = 2πbdb leave the scattering area at a solid angle dΩ = 2π sin(χ)dχ. The differential cross section is then defined as: dσ b ∂b I(Ω) = = dΩ sin(χ) ∂χ

ra b 6 ?

ϕ

χ M

For a potential energy W (r) = kr−n follows: I(Ω, v) ∼ v −4/n . For low energies, O(1 eV), σ has a Ramsauer minimum. It arises from the interference of matter waves behind the object. I(Ω) for angles 0 < χ < λ/4 is larger than the classical value.

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56

11.3.2 The Coulomb interaction For the Coulomb interaction holds: 2b0 = q1 q2 /2πε0 mv02 , so W (r) = 2b0 /r. This gives b = b0 cot( 12 χ) and b20 b ∂b = sin(χ) ∂χ 4 sin2 ( 12 χ)

I(Ω =

Because the influence of a particle vanishes at r = λD holds: σ = π(λ2D − b20 ). Because dp = d(mv) = mv0 (1 − cos χ) a cross section related to momentum transfer σm is given by: 

Z (1 − cos χ)I(Ω)dΩ = 4πb20 ln

σm =

1 sin( 12 χmin )



 = 4πb20 ln

λD b0

 := 4πb20 ln(ΛC ) ∼

ln(v 4 ) v4

where ln(ΛC ) is the Coulomb-logarithm. For this quantity holds: ΛC = λD /b0 = 9n(λD ).

11.3.3 The induced dipole interaction ~ gives a potential V and an energy W in a dipole field given by: The induced dipole interaction, with ~ p = αE, V (r) = s with ba =

4

|e|p αe2 p~ · ~er , W (r) = − = − 4πε0 r2 8πε0 r2 2(4πε0 )2 r4

2e2 α holds: χ = π − 2b (4πε0 )2 12 mv02

Z∞ r ra

r2

dr

1−

b2 b4 + a4 2 r 4r

If b ≥ ba the charge would hit the atom. Repulsing nuclear forces prevent this to happen. If the scattering angle is a lot times 2π it is called capture. The cross section for capture σorb = πb2a is called the Langevin limit, and is a lowest estimate for the total cross section.

11.3.4 The centre of mass system If collisions of two particles with masses m1 and m2 which scatter in the centre of mass system by an angle χ are compared with the scattering under an angle θ in the laboratory system holds: tan(θ) =

m2 sin(χ) m1 + m2 cos(χ)

The energy loss ∆E of the incoming particle is given by: ∆E = E

1 2 2 m2 v2 1 2 2 m1 v1

=

2m1 m2 (1 − cos(χ)) (m1 + m2 )2

11.3.5 Scattering of light Scattering of light by free electrons is called Thomson scattering. The scattering is free from collective effects if kλD  1. The cross section σ = 6.65 · 10−29 m2 and 2v ∆f = sin( 12 χ) f c This gives for the scattered energy Escat ∼ nλ40 /(λ2 − λ20 )2 with n the density. If λ  λ0 it is called Rayleigh scattering. Thomson sccattering is a limit of Compton scattering, which is given by λ0 − λ = λC (1 − cos χ) with λC = h/mc and cannot be used any more if relativistic effects become important.

Chapter 11: Plasma physics

57

11.4 Thermodynamic equilibrium and reversibility Planck’s radiation law and the Maxwellian velocity distribution hold for a plasma in equilibrium:   2πn √ E 1 8πhν 3 dν , N (E, T )dE = E exp − dE ρ(ν, T )dν = c3 exp(hν/kT ) − 1 kT (πkT )3/2 “Detailed balancing” means that the number of reactions in one direction equals the number of reactions in the opposite direction because both processes have equal probability if one corrects for the used phase space. For the reaction X X Xforward → Xback ← forward

back

holds in a plasma in equilibrium microscopic reversibility: Y Y ηˆforward = ηˆback forward

back

If the velocity distribution is Maxwellian, this gives: ηˆx =

nx h3 e−Ekin /kT gx (2πmx kT )3/2

where g is the statistical weight of the state and n/g := η. For electrons holds g = 2, for excited states usually holds g = 2j + 1 = 2n2 . With this one finds for the Boltzmann balance, Xp + e− → ← X1 + e− + (E1p ): nB gp p = exp n1 g1



Ep − E1 kTe



+ And for the Saha balance, Xp + e− + (Epi ) → ← X1 + 2e− :

nSp n+ h3 1 ne = + exp gp g1 ge (2πme kTe )3/2



Epi kTe



Because the number of particles on the left-hand side and right-hand side of the equation is different, a factor g/Ve remains. This factor causes the Saha-jump. From microscopic reversibility one can derive that for the rate coefficients K(p, q, T ) := hσvipq holds: K(q, p, T ) =

  ∆Epq gp K(p, q, T ) exp gq kT

11.5 Inelastic collisions 11.5.1 Types of collisions The kinetic energy can be split in a part of and a part in the centre of mass system. The energy in the centre of mass system is available for reactions. This energy is given by E=

m1 m2 (v1 − v2 )2 2(m1 + m2 )

Some types of inelastic collisions important for plasma physics are: 1. Excitation: Ap + e− → ← Aq + e− 2. Decay: Aq → ← Ap + hf

Physics Formulary by ir. J.C.A. Wevers

58

3. Ionisation and 3-particles recombination: Ap + e− → ← A+ + 2e− 4. radiative recombination: A+ + e− → ← Ap + hf 5. Stimulated emission: Aq + hf → Ap + 2hf 6. Associative ionisation: A∗∗ + B → ← AB+ + e− 7. Penning ionisation: b.v. Ne∗ + Ar → ← Ar+ + Ne + e− 8. Charge transfer: A+ + B → ← A + B+ 9. Resonant charge transfer: A+ + A → ← A + A+

11.5.2 Cross sections Collisions between an electron and an atom can be approximated by a collision between an electron and one of the electrons of that atom. This results in πZ 2 e4 dσ = d(∆E) (4πε0 )2 E(∆E)2 Then follows for the transition p → q: σpq (E) =

πZ 2 e4 ∆Eq,q+1 (4πε0 )2 E(∆E)2pq

For ionization from state p holds to a good approximation: σp = For resonant charge transfer holds: σex =



4πa20 Ry

1 1 − Ep E



 ln

1.25βE Ep



A[1 − B ln(E)]2 1 + CE 3.3

11.6 Radiation In equilibrium holds for radiation processes: np Apq + np Bpq ρ(ν, T ) = nq Bqp ρ(ν, T ) | {z } {z } {z } | | emission

stimulated emission

absorption

Here, Apq is the matrix element of the transition p → q, and is given by: 8π 2 e2 ν 3 |rpq |2 with rpq = hψp |~r |ψq i 3¯ hε0 c3 P For hydrogenic atoms holds: Ap = 1.58 · 108 Z 4 p−4.5 , with Ap = 1/τp = Apq . The intensity I of a line is Apq =

q

given by Ipq = hf Apq np /4π. The Einstein coefficients B are given by: Bpq =

c3 Apq Bpq gq and = 8πhν 3 Bqp gp

A spectral line is broadened by several mechanisms: 1. Because the states have a finite life time. The natural life time of a state p is given by τp = 1/

P q

From the uncertainty relation then follows: ∆(hν) · τp = 12 ¯h, this gives P Apq 1 q = ∆ν = 4πτp 4π The natural line width is usually  than the broadening due to the following two mechanisms:

Apq .

Chapter 11: Plasma physics

59

2. The Doppler broadening is caused by the thermal motion of the particles: s 2 2 ln(2)kTi ∆λ = λ c mi This broadening results in a Gaussian line profile: √ kν = k0 exp(−[2 ln 2(ν − ν0 )/∆νD ]2 ), with k the coefficient of absorption or emission. 3. The Stark broadening is caused by the electric field of the electrons:  ∆λ1/2 =

ne C(ne , Te )

2/3

˚ −3/2 cm−3 . with for the H-β line: C(ne , Te ) ≈ 3 · 1014 A The natural broadening and the Stark broadening result in a Lorentz profile of a spectral line: kν = 12 k0 ∆νL /[( 21 ∆νL )2 + (ν − ν0 )2 ]. The total line shape is a convolution of the Gauss- and Lorentz profile and is called a Voigt profile. The number of transitions p → q is given by np Bpq ρ and by np nhf hσa ci = np (ρdν/hν)σa c where dν is the line width. Then follows for the cross section of absorption processes: σa = Bpq hν/cdν. The background radiation in a plasma originates from two processes: 1. Free-Bound radiation, originating from radiative recombination. The emission is given by:    C1 zi ni ne hc 1 − exp − ξf b (λ, Te ) εf b = 2 √ λ λkTe kTe with C1 = 1.63 · 10−43 Wm4 K1/2 sr−1 and ξ the Biberman factor. 2. Free-free radiation, originating from the acceleration of particles in the EM-field of other particles:   C1 zi ni ne hc exp − ξf f (λ, Te ) εf f = 2 √ λ λkTe kTe

11.7 The Boltzmann transport equation It is assumed that there exists a distribution function F for the plasma so that F (~r, ~v , t) = Fr (~r, t) · Fv (~v , t) = F1 (x, t)F2 (y, t)F3 (z, t)F4 (vx , t)F5 (vy , t)F6 (vz , t)   ∂F ∂F dF = + ∇r · (F~v ) + ∇v · (F~a ) = Then the BTE is: dt ∂t ∂t coll−rad Assuming that v does not depend on r and ai does not depend on vi , holds ∇r ·(F~v ) = ~v ·∇F and ∇v ·(F~a ) = is separated in a thermal ~a · ∇v F . This is also true in magnetic fields because ∂ai /∂xi = R0. The velocity R ~ The total density is given by n = F d~v and ~v F d~v = nw. ~ velocity ~vt and a drift velocity w. The balance equations can be derived by means of the moment method:   Z ∂n ∂n + ∇ · (nw) ~ = 1. Mass balance: (BTE)d~v ⇒ ∂t ∂t cr Z dw ~ ~ + ∇T0 + ∇p = mn h~a i + R 2. Momentum balance: (BTE)m~v d~v ⇒ mn dt Z 3 dp 5 + p∇ · w ~ + ∇ · ~q = Q 3. Energy balance: (BTE)mv 2 d~v ⇒ 2 dt 2

Physics Formulary by ir. J.C.A. Wevers

60

 ~ +w ~ ) is the average acceleration, ~q = 1 nm ~v 2~vt the heat flow, Here, h~a i = e/m(E ~ ×B t 2   Z mvt2 ∂F ~ is a friction term and p = nkT the d~v the source term for energy production, R Q = r ∂t cr pressure. X e2 (ne + zi ni ) pi − A thermodynamic derivation gives for the total pressure: p = nkT = 24πε0 λD i For the electrical conductance in a plasma follows from the momentum balance, if we  wi : ~− η J~ = E

~ + ∇pe J~ × B ene

In a plasma where only elastic e-a collisions are important the equilibrium energy distribution function is the Druyvesteyn distribution: "  3/2  2 # E 3me E exp − dE N (E)dE = Cne E0 m0 E0 with E0 = eEλv = eE/nσ.

11.8 Collision-radiative models These models are first-moment equations for excited states. One assumes the Quasi-steady-state solution is ~ p ) = 0)]. This results in: valid, where ∀p>1 [(∂np /∂t = 0) ∧ (∇ · (np w       ∂n1 ∂ni ∂n1 ∂ni ∂np>1 + ∇ · (n1 w + ∇ · (ni w =0 , ~ 1) = , ~ i) = ∂t ∂t ∂t cr ∂t ∂t cr cr S with solutions np = rp0 nSp +rp1 nB p = bp np . Further holds for all collision-dominated levels that δbp := bp −1 = p Ry/Epi and 5 ≤ x ≤ 6. For systems in ESP, where only collisional (de)excitation b0 p−x eff with peff = between levels p and p ± 1 is taken into account holds x = 6. Even in plasma’s far from equilibrium the excited levels will eventually reach ESP, so from a certain level up the level densities can be calculated.

To find the population densities of the lower levels in the stationary case one has to start with a macroscopic equilibrium: Number of populating processes of level p = Number of depopulating processes of level p , When this is expanded it becomes: X X X nq Kqp + ne nq Kqp + nq Aqp + n2e ni K+p + ne ni αrad = ne | {z } | {z } q

p q>p | {z } | {z } | {z } coll. recomb. rad. recomb coll. excit.

n e np |

coll. deexcit.

X

Kpq + ne np

q
{z

}

coll. deexcit.

|

rad. deex. to

X

Kpq + np

q>p

{z

coll. excit.

}

|

X

Apq + ne np Kp+ | {z } coll. ion. {z }

q
rad. deex. from

11.9 Waves in plasma’s Interaction of electromagnetic waves in plasma’s results in scattering and absorption of energy. For electromagnetic waves with complex wave number k = ω(n + iκ)/c in one dimension one finds: Ex = E0 e−κωx/c cos[ω(t − nx/c)]. The refractive index n is given by: r ωp2 c k = 1− 2 n=c = ω vf ω

Chapter 11: Plasma physics

61

~ˆ i(kz−ωt) ~ = B0~ez + Be For disturbances in the z-direction in a cold, homogeneous, magnetized plasma: B and i(kz−ωt) ˆe (external E fields are screened) follows, with the definitions α = ωp /ω and β = Ω/ω n = n0 + n 2 2 + ωpe : and ωp2 = ωpi  ~ , with ~ J~ = ~ ~σ E ~σ = iε0 ω

X s

  α2s  

1 1 − βs2 iβs 1 − βs2 0

−iβs 1 − βs2 1 1 − βs2 0

 0

  0   1

where the sum is taken over particle species s. The dielectric tensor E, with property: ~k · (~E~ · E) ~ =0 ~ ~ ~σ /iε0 ω. is given by E~ = I~ − ~ With the definitions S = 1 −

X s

X α2 βs X α2s s , D= , P =1− α2s 2 2 1 − βs 1 − β s s s 

follows:

S ~~  iD E= 0

−iD S 0

 0 0  P

The √ eigenvalues of this √ hermitian matrix are R = S + D, L = S − D, λ3 = P , with eigenvectors ~er = 1 1 2(1, i, 0), ~ e = e3 = (0, 0, 1). ~er is connected with a right rotating field for which l 2 2 2(1, −i, 0) and ~ iEx /Ey = 1 and ~el is connected with a left rotating field for which iEx /Ey = −1. When k makes an angle θ ~ one finds: with B P (n2 − R)(n2 − L) tan2 (θ) = S(n2 − RL/S)(n2 − P ) where n is the refractive index. From this the following solutions can be obtained: A. θ = 0: transmission in the z-direction. 1. P = 0: Ex = Ey = 0. This describes a longitudinal linear polarized wave. 2. n2 = L: a left, circular polarized wave. 3. n2 = R: a right, circular polarized wave. B. θ = π/2: transmission ⊥ the B-field. 1. n2 = P : the ordinary mode: Ex = Ey = 0. This is a transversal linear polarized wave. 2. n2 = RL/S: the extraordinary mode: iEx /Ey = −D/S, an elliptical polarized wave. Resonance frequencies are frequencies for which n2 → ∞, so vf = 0. For these holds: tan(θ) = −P/S. For R → ∞ this gives the electron cyclotron resonance frequency ω = Ωe , for L → ∞ the ion cyclotron resonance frequency ω = Ωi and for S = 0 holds for the extraordinary mode:      mi Ω2i m2i Ω2i Ω2i = 1 − 1 − α2 1 − me ω 2 m2e ω 2 ω2 Cut-off frequencies are frequencies for which n2 = 0, so vf → ∞. For these holds: P = 0 or R = 0 or L = 0. In the case that β 2  1 one finds Alfv´en waves propagating parallel to the field lines. With the Alfv´en velocity vA = follows: n =

Ωe Ωi 2 2 c + ωpi

2 ωpe

p 1 + c/vA , and in case vA  c: ω = kvA .

Chapter 12

Solid state physics 12.1 Crystal structure A lattice is defined by the 3 translation vectors ~ai , so that the atomic composition looks the same from each point ~r and ~r0 = ~r + T~ , where T~ is a translation vector given by: T~ = u1~a1 + u2~a2 + u3~a3 with ui ∈ IN . A lattice can be constructed from primitive cells. As a primitive cell one can take a parallellepiped, with volume Vcell = |~a1 · (~a2 × ~a3 )| Because a lattice has a periodical structure the physical properties which are connected with the lattice have the same periodicity (neglecting boundary effects): ne (~r + T~ ) = ne (~r ) This periodicity is suitable to use Fourier analysis: n(~r ) is expanded as: X ~ · ~r ) nG exp(iG n(~r ) = G

with nG =

1

ZZZ ~ · ~r )dV n(~r ) exp(−iG

Vcell cell

~ is the reciprocal lattice vector. If G ~ is written as G ~ = v1~b1 + v2~b2 + v3~b3 with vi ∈ IN , it follows for the G vectors ~bi , cyclically: ~bi = 2π ~ai+1 × ~ai+2 ~ai · (~ai+1 × ~ai+2 ) ~ The set of G-vectors determines the R¨ontgen diffractions: a maximum in the reflected radiation occurs if: ~ ~ = G2 . From this follows for parallel lattice planes (Bragg reflection) ~ ∆k = G with ∆~k = ~k − ~k 0 . So: 2~k · G that for the maxima holds: 2d sin(θ) = nλ. The Brillouin zone is defined as a Wigner-Seitz cell in the reciprocal lattice.

12.2 Crystal binding A distinction can be made between 4 binding types: 1. Van der Waals bond 2. Ion bond 3. Covalent or homopolar bond 4. Metalic bond. For the ion binding of NaCl the energy per molecule is calculated by: E = cohesive energy(NaCl) – ionization energy(Na) + electron affinity(Cl) The interaction in a covalent bond depends on the relative spin orientations of the electrons constituing the bond. The potential energy for two parallel spins is higher than the potential energy for two antiparallel spins. Furthermore the potential energy for two parallel spins has sometimes no minimum. In that case binding is not possible. 62

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63

12.3 Crystal vibrations 12.3.1 A lattice with one type of atoms In this model for crystal vibrations only nearest-neighbour interactions are taken into account. The force on atom s with mass M can then be written as: Fs = M

d2 us = C(us+1 − us ) + C(us−1 − us ) dt2

Assuming that all solutions have the same time-dependence exp(−iωt) this results in: −M ω 2 us = C(us+1 + us−1 − 2us ) Further it is postulated that: us±1 = u exp(isKa) exp(±iKa). This gives: us = exp(iKsa). Substituting the later two equations in the fist results in a system of linear equations, which has only a solution if their determinant is 0. This gives: ω2 =

4C sin2 ( 12 Ka) M

Only vibrations with a wavelength within the first Brillouin Zone have a physical significance. This requires that −π < Ka ≤ π. The group velocity of these vibrations is given by: dω = vg = dK

r

Ca2 cos( 12 Ka) . M

and is 0 on the edge of a Brillouin Zone. Here, there is a standing wave.

12.3.2 A lattice with two types of atoms ω 6

Now the solutions are:  2

ω =C

1 1 + M1 M2

s

 ±C

1 1 + M1 M2

2 −

4 sin2 (Ka) M1 M2

Connected with each value of K are two values of ω, as can be seen in the graph. The upper line describes the optical branch, the lower line the acoustical branch. In the optical branch, both types of ions oscillate in opposite phases, in the acoustical branch they oscillate in the same phase. This results in a much larger induced dipole moment for optical oscillations, and also a stronger emission and absorption of radiation. Furthermore each branch has 3 polarization directions, one longitudinal and two transversal.

q q

0

2C M2 2C M1

- K π/a

12.3.3 Phonons The quantum mechanical excitation of a crystal vibration with an energy ¯hω is called a phonon. Phonons can be viewed as quasi-particles: with collisions, they behave as particles with momentum ¯hK. Their total momentum is 0. When they collide, their momentum need not be conserved: for a normal process holds: K1 + K2 = K3 , for an umklapp process holds: K1 + K2 = K3 + G. Because phonons have no spin they behave like bosons.

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12.3.4 Thermal heat capacity The total energy of the crystal vibrations can be calculated by multiplying each mode with its energy and sum over all branches K and polarizations P : XZ XX ¯hω dω hω hnk,p i = ¯ Dλ (ω) U= exp(¯hω/kT ) − 1 K

P

λ

for a given polarization λ. The thermal heat capacity is then: XZ ∂U (¯hω/kT )2 exp(¯hω/kT ) =k dω D(ω) Clattice = ∂T (exp(¯hω/kT ) − 1)2 λ

The dispersion relation in one dimension is given by: D(ω)dω =

L dω L dK dω = π dω π vg

In three dimensions one applies periodic boundary conditions to a cube with N 3 primitive cells and a volume L3 : exp(i(Kx x + Ky y + Kz z)) ≡ exp(i(Kx (x + L) + Ky (y + L) + Kz (z + L))). Because exp(2πi) = 1 this is only possible if: Kx , Ky , Kz = 0; ±

4π 6π 2N π 2π ; ± ; ± ; ... ± L L L L

~ per volume (2π/L)3 in K-space, or: So there is only one allowed value of K  3 V L = 2π 8π 3 ~ ~ allowed K-values per unit volume in K-space, for each polarization and each branch. The total number of states with a wave vector < K is:  3 4πK 3 L N= 2π 3 for each polarization. The density of states for each polarization is, according to the Einstein model:   ZZ V K 2 dK V dAω dN = = D(ω) = dω 2π 2 dω 8π 3 vg The Debye model for thermal heat capacities is a low-temperature approximation which is valid up to ≈ 50K. Here, only the acoustic phonons are taken into account (3 polarizations), and one assumes that v = ωK, independent of the polarization. From this follows: D(ω) = V ω 2 /2π 2 v 3 , where v is the speed of sound. This gives: ZωD ZxD 3 Z 3V k 2 T 4 V ω2 ¯hω x dx dω = . U = 3 D(ω) hni ¯ hωdω = 3 x −1 2 3 2π 2 v 3 exp(¯hω/kT ) − 1 e 2π v ¯h 0

0

¯ ωD /kT = θD /T . θD is the Debye temperature and is defined by: Here, xD = h θD =

¯v h k



6π 2 N V

1/3

where N is the number of primitive cells. Because xD → ∞ for T → 0 it follows from this:  U = 9N kT

T θD

3 Z∞ 0

3π 4 N kT 4 12π 4 N kT 3 x3 dx = ∼ T 4 and CV = ∼ T3 3 x e −1 5θD 5θD

In the Einstein model for the thermal heat capacity one considers only phonons at one frequency, an approximation for optical phonons.

Chapter 12: Solid state physics

65

12.4 Magnetic field in the solid state The following graph shows the magnetization versus fieldstrength for different types of magnetism: M 6 Msat χm

ferro

∂M = ∂H

paramagnetism

0 hhhh hhh hhdiamagnetism hh h

- H

12.4.1 Dielectrics The quantum mechanical origin of diamagnetism is the Larmorprecession of the spin of the electron. Starting with a circular electron orbit in an atom with two electrons, there is a Coulomb force Fc and a magnetic force on each electron. If the magnetic part of the force is not strong enough to significantly deform the orbit holds: s 2 Fc (r) eB eB eB eB 2 2 ± ω = ω0 ± (ω0 + δ) ⇒ ω = = ω0 ± ωL + · · · ≈ ω0 ± ω0 ± ω = mr m m 2m 2m Here, ωL is the Larmor frequency. One electron is accelerated, the other decelerated. Hence there is a net circular current which

 results in amagnetic moment ~µ. The circular current is given by I = −ZeωL /2π, and hµi = IA = Iπ ρ2 = 23 Iπ r2 . If N is the number of atoms in the crystal it follows for the susceptibility, ~ = ~µN : with M µ0 N Ze2 2  µ0 M =− r χ= B 6m

12.4.2 Paramagnetism ~ = mJ gµB B, and with a Starting with the splitting of energy levels in a weak magnetic field: ∆Um − ~µ · B P P /kT ), one finds for the average magnetic moment hµi = fm µ/ fm . After distribution fm ∼ exp(−∆U P P 2 Pm linearization and because mJ = 0, J = 2J + 1 and mJ = 23 J(J + 1)(J + 12 ) it follows that: χp =

µ0 N hµi µ0 J(J + 1)g 2 µ2B N µ0 M = = B B 3kT

This is the Curie law, χp ∼ 1/T .

12.4.3 Ferromagnetism A ferromagnet behaves like a paramagnet above a critical temperature Tc . To describe ferromagnetism a field ~ . From there the treatment is analogous to the paramagnetic ~ E = λµ0 M BE parallel with M is postulated: B case:   C M µ0 M = χp (Ba + BE ) = χp (Ba + λµ0 M ) = µ0 1 − λ T From this follows for a ferromagnet: χF =

µ0 M C = which is Weiss-Curie’s law. Ba T − Tc

If BE is estimated this way it results in values of about 1000 T. This is clearly unrealistic and suggests another mechanism. A quantum mechanical approach from Heisenberg postulates an interaction between two neigh~j ≡ −~ ~ E . J is an overlap integral given by: J = 3kTc /2zS(S + 1), with ~i · S µ·B bouring atoms: U = −2J S z the number of neighbours. A distinction between 2 cases can now be made: 1. J > 0: Si and Sj become parallel: the material is a ferromagnet.

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2. J < 0: Si and Sj become antiparallel: the material is an antiferromagnet. Heisenberg’s theory predicts quantized spin waves: magnons. Starting from a model with only nearest neighbouring atoms interacting one can write: ~p−1 + S ~p+1 ) ≈ ~µp · B ~ p with B ~ p = −2J (S ~p−1 + S ~p+1 ) ~p · (S U = −2J S gµB The equation of motion for the magnons becomes:

~ 2J ~ dS ~p−1 + S ~p+1 ) = Sp × (S dt ¯ h

~p = ~u exp(i(pka − From here the treatment is analogous to phonons: postulate traveling waves of the type S ωt)). This results in a system of linear equations with solution: ¯hω = 4JS(1 − cos(ka))

12.5 Free electron Fermi gas 12.5.1 Thermal heat capacity The solution with period L of the one-dimensional Schr¨odinger equation is: ψn (x) = A sin(2πx/λn) with nλn = 2L. From this follows ¯h2  nπ 2 E= 2m L In a linear lattice the only important quantum numbers are n and ms . The Fermi level is the uppermost filled level in the ground state, which has the Fermi-energy EF . If nF is the quantum number of the Fermi level, it ¯ 2 π 2 N 2 /8mL. In 3 dimensions holds: can be expressed as: 2nF = N so EF = h  kF =

3π 2 N V

1/3 and EF =

¯2 h 2m



3π 2 N V

2/3

 3/2 2mE V The number of states with energy ≤ E is then: N = . 3π 2 ¯h2  3/2 √ V 2m 3N dN = . E= and the density of states becomes: D(E) = 2 2 dE 2π 2E ¯h The heat capacity of the electrons is approximately 0.01 times the classical expected value 32 N k. This is caused by the Pauli exclusion principle and the Fermi-Dirac distribution: only electrons within an energy range ∼ kT of the Fermi level are excited thermally. There is a fraction ≈ T /TF excited thermally. The internal energy then becomes: T ∂U T ≈ Nk and C = U ≈ N kT TF ∂T TF A more accurate analysis gives: Celectrons = 12 π 2 N kT /TF ∼ T . Together with the T 3 dependence of the thermal heat capacity of the phonons the total thermal heat capacity of metals is described by: C = γT + AT 3 .

12.5.2 Electric conductance The equation of motion for the charge carriers is: F~ = md~v /dt = h ¯ d~k/dt. The variation of ~k is given by ~ h. If τ is the characteristic collision time of the electrons, δ~k remains stable if δ~k = ~k(t) − ~k(0) = −eEt/¯ ~ with µ = eτ /m the mobility of the electrons. t = τ . Then holds: h~v i = µE, ~ = E/ρ ~ = neµE. ~ Because for the collision time holds: The current in a conductor is given by: J~ = nq~v = σ E 1/τ = 1/τL + 1/τi , where τL is the collision time with the lattice phonons and τi the collision time with the impurities follows for the resistivity ρ = ρL + ρi , with lim ρL = 0. T →0

Chapter 12: Solid state physics

67

12.5.3 The Hall-effect If a magnetic field is applied ⊥ to the direction of the current the charge carriers will be pushed aside by the ~ = B~ez Lorentz force. This results in a magnetic field ⊥ to the flow direction of the current. If J~ = J~ex and B than Ey /Ex = µB. The Hall coefficient is defined by: RH = Ey /Jx B, and RH = −1/ne if Jx = neµEx . The Hall voltage is given by: VH = Bvb = IB/neh where b is the width of the material and h de height.

12.5.4 Thermal heat conductivity With ` = vF τ the mean free path of the electrons follows from κ = 13 C hvi `: κelectrons = π 2 nk 2 T τ /3m. From this follows for the Wiedemann-Franz ratio: κ/σ = 13 (πk/e)2 T .

12.6 Energy bands In the tight-bond approximation it is assumed that ψ = eikna φ(x − na). From this follows for the energy: hEi = hψ|H|ψi = Eat − α − 2β cos(ka). So this gives a cosine superimposed on the atomic energy, which can often be approximated by a harmonic oscillator. If it is assumed that the electron is nearly free one can postulate: ψ = exp(i~k · ~r ). This is a traveling wave. This wave can be decomposed into two standing waves: ψ(+) = ψ(−) =

exp(iπx/a) + exp(−iπx/a) = 2 cos(πx/a) exp(iπx/a) − exp(−iπx/a) = 2i sin(πx/a)

The probability density |ψ(+)|2 is high near the atoms of the lattice and low in between. The probability density |ψ(−)|2 is low near the atoms of the lattice and high in between. Hence the energy of ψ(+) is also lower than the energy of ψ)(−). Suppose that U (x) = U cos(2πx/a), than the bandgap is given by: Z1 Egap =

  U (x) |ψ(+)|2 − |ψ(−)|2 dx = U

0

12.7 Semiconductors The band structures and the transitions between them of direct and indirect semiconductors are shown in the figures below. Here it is assumed that the momentum of the absorbed photon can be neglected. For an indirect semiconductor a transition from the valence- to the conduction band is also possible if the energy of the absorbed photon is smaller than the band gap: then, also a phonon is absorbed. conduction E band 6 •  6  ωg   ◦

Direct transition This difference can also be observed in the absorption spectra:

E 6 • Ω

6 ω   ◦

Indirect transition

Physics Formulary by ir. J.C.A. Wevers

68

absorption

absorption

6

6 . ... . . .. ... . .

.

....

.. ¯Ω Eg + h

-E

hω g ¯

Direct semiconductor

- E

Indirect semiconductor

So indirect semiconductors, like Si and Ge, cannot emit any light and are therefore not usable to fabricate lasers. When light is absorbed holds: ~kh = −~ke , Eh (~kh ) = −Ee (~ke ), ~vh = ~ve and mh = −m∗e if the conduction band and the valence band have the same structure. Instead of the normal electron mass one has to use the effective mass within a lattice. It is defined by:  2 −1 dp/dt dK F d E 2 ∗ = =h ¯ =h ¯ m = a dvg /dt dvg dk 2 with E = h ¯ ω and vg = dω/dk and p = h ¯ k. With the distribution function fe (E) ≈ exp((µ − E)/kT ) for the electrons and fh (E) = 1 − fe (E) for the holes the density of states is given by:  3/2 p 2m∗ 1 E − Ec D(E) = 2π 2 ¯h2 with Ec the energy at the edge of the conductance band. From this follows for the concentrations of the holes p and the electrons n: 

Z∞ De (E)fe (E)dE = 2

n=

m∗ kT 2π¯h2



3/2 exp

µ − Ec kT



Ec

  3 p E kT ∗ m exp − g m e h kT 2π¯ h2 For an intrinsic (no impurities) semiconductor holds: ni = pi , for a n − type holds: n > p and in a p − type holds: n < p. 

For the product np follows: np = 4

An exciton is a bound electron-hole pair, rotating on each other as in positronium. The excitation energy of an exciton is smaller than the bandgap because the energy of an exciton is lower than the energy of a free electron and a free hole. This causes a peak in the absorption just under Eg .

12.8 Superconductivity 12.8.1 Description A superconductor is characterized by a zero resistivity if certain quantities are smaller than some critical values: T < Tc , I < Ic and H < Hc . The BCS-model predicts for the transition temperature Tc :   −1 Tc = 1.14ΘD exp U D(EF ) while experiments find for Hc approximately:

  T2 Hc (T ) ≈ Hc (Tc ) 1 − 2 . Tc

Chapter 12: Solid state physics

69

Within a superconductor the magnetic field is 0: the Meissner effect. There are type I and type II superconductors. Because the Meissner effect implies that a superconductor is a ~ . This holds for a type I superconductor, for ~ = µ0 M perfect diamagnet holds in the superconducting state: H a type II superconductor this only holds to a certain value Hc1 , for higher values of H the superconductor is in a vortex state to a value Hc2 , which can be 100 times Hc1 . If H becomes larger than Hc2 the superconductor becomes a normal conductor. This is shown in the figures below. µ0 M

µ0 M

6

6

Hc

-H

·· ·· ·· ·· ·· ·· ·· · Hc1

Type I

- H Hc2 Type II

The transition to a superconducting state is a second order thermodynamic state transition. This means that there is a twist in the T − S diagram and a discontinuity in the CX − T diagram.

12.8.2 The Josephson effect For the Josephson effect one considers two superconductors, separated by an insulator. The electron wavefunction in one superconductor is ψ1 , in the other ψ2 . The Schr¨odinger equations in both superconductors is set equal: ∂ψ2 ∂ψ1 =h ¯ T ψ2 , i¯h =h ¯ T ψ1 i¯ h ∂t ∂t ¯ T is the effect of the coupling of the electrons, or the transfer interaction through the insulator. The electron h √ √ wavefunctions are written √ as ψ1 = n1 exp(iθ1 ) and ψ2 = n2 exp(iθ2 ). Because a Cooper pair exist of two electrons holds: ψ ∼ n. From this follows, if n1 ≈ n2 : ∂θ2 ∂n2 ∂n1 ∂θ1 = and =− ∂t ∂t ∂t ∂t The Josephson effect results in a current density through the insulator depending on the phase difference as: J = J0 sin(θ2 − θ1 ) = J0 sin(δ), where J0 ∼ T . With an AC-voltage across the junction the Schr¨odinger equations become: ∂ψ2 ∂ψ1 =h ¯ T ψ2 − eV ψ1 and i¯h =h ¯ T ψ1 + eV ψ2 i¯ h ∂t ∂t   2eV t This gives: J = J0 sin θ2 − θ1 − . h ¯ Hence there is an oscillation with ω = 2eV /¯h.

12.8.3 Flux quantisation in a superconducting ring nq ~ ~] [¯ h∇θ − q A m H ~ = 0 and J~ = 0, follows: ¯h∇θ ~ = qA ~ ⇒ ∇θdl ~ From the Meissner effect, B = θ2 − θ1 = 2πs with s ∈ IN . H RR RR ~ = (rotA, ~ ~n )dσ = (B, ~ ~n )dσ = Ψ follows: Ψ = 2π¯hs/q. The size of a flux quantum Because: Adl follows by setting s = 1: Ψ = 2π¯ h/e = 2.0678 · 10−15 Tm2 . For the current density in general holds: J~ = qψ ∗~v ψ =

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12.8.4 Macroscopic quantum interference 2eΨ , so From θ2 − θ1 = 2eΨ/¯ h follows for two parallel junctions: δb − δa = ¯h    eΨ This gives maxima if eΨ/¯h = sπ. J = Ja + Jb = 2J0 sin δ0 cos h ¯

12.8.5 The London equation ~ is postulated: A current density in a superconductor proportional to the vector potential A ~ ~ −B −A or rotJ~ = J~ = 2 µ0 λL µ0 λ2L where λL =

p ~ = B/λ ~ 2. ε0 mc2 /nq 2 . From this follows: ∇2 B L

~ The Meissner effect is the solution of this equation: B(x) = B0 exp(−x/λL ). Magnetic fields within a superconductor drop exponentially.

12.8.6 The BCS model The BCS model can explain superconductivity in metals. (So far there is no explanation for high-Tc superconductance). A new ground state where the electrons behave like independent fermions is postulated. Because of the interaction with the lattice these pseudo-particles exhibit a mutual attraction. This causes two electrons with opposite spin to combine to a Cooper pair. It can be proved that this ground state is perfect diamagnetic. The infinite conductivity is more difficult to explain because a ring with a persisting current is not a real equilibrium: a state with zero current has a lower energy. Flux quantization prevents transitions between these states. Flux quantization is related to the existence of a coherent many-particle wavefunction. A flux quantum is the equivalent of about 104 electrons. So if the flux has to change with one flux quantum there has to occur a transition of many electrons, which is very improbable, or the system must go through intermediary states where the flux is not quantized so they have a higher energy. This is also very improbable. Some useful mathematical relations are: Z∞

π2 xdx = , ax e +1 12a2

0

And, when

∞ X

Z∞ −∞

π2 x2 dx , = x 2 (e + 1) 3

Z∞ n

(−1) =

n=0

1 2

0

Z∞ sin(px)dx =

follows: 0

Z∞

cos(px)dx = 0

1 . p

π4 x3 dx = x e +1 15

Chapter 13

Theory of groups 13.1 Introduction 13.1.1 Definition of a group G is a group for the operation • if: 1. ∀A,B∈G ⇒ A • B ∈ G: G is closed. 2. ∀A,B,C∈G ⇒ (A • B) • C = A • (B • C): G obeys the associative law. 3. ∃E∈G so that ∀A∈G A • E = E • A = A: G has a unit element. 4. ∀A∈G ∃A−1 ∈G so that A • A−1 = E: Each element in G has an inverse. If also holds: 5. ∀A,B∈G ⇒ A • B = B • A the group is called Abelian or commutative.

13.1.2 The Cayley table Each element arises only once in each row and column of the Cayley- or multiplication table: because EAi = A−1 k (Ak Ai ) = Ai each Ai appears once. There are h positions in each row and column when there are h elements in the group so each element appears only once.

13.1.3 Conjugated elements, subgroups and classes B is conjugate to A if ∃X∈G such that B = XAX −1 . Then A is also conjugate to B because B = (X −1 )A(X −1 )−1 . If B and C are conjugate to A, B is also conjugate with C. A subgroup is a subset of G which is also a group w.r.t. the same operation. A conjugacy class is the maximum collection of conjugated elements. Each group can be split up in conjugacy classes. Some theorems: • All classes are completely disjoint. • E is a class itself: for each other element in this class would hold: A = XEX −1 = E. • E is the only class which is also a subgroup because all other classes have no unit element. • In an Abelian group each element is a separate class. The physical interpretation of classes: elements of a group are usually symmetry operations which map a symmetrical object into itself. Elements of one class are then the same kind of operations. The opposite need not to be true. 71

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72

13.1.4 Isomorfism and homomorfism; representations Two groups are isomorphic if they have the same multiplication table. The mapping from group G1 to G2 , so that the multiplication table remains the same is a homomorphic mapping. It need not be isomorphic. A representation is a homomorphic mapping of a group to a group of square matrices with the usual matrix multiplication as the combining operation. This is symbolized by Γ. The following holds: Γ(E) = II , Γ(AB) = Γ(A)Γ(B) , Γ(A−1 ) = [Γ(A)]−1 For each group there are 3 possibilities for a representation: 1. A faithful representation: all matrices are different. 2. The representation A → det(Γ(A)). 3. The identical representation: A → 1. An equivalent representation is obtained by performing an unitary base transformation: Γ0 (A) = S −1 Γ(A)S.

13.1.5 Reducible and irreducible representations If the same unitary transformation can bring all matrices of a representation Γ in the same block structure the representation is called reducible:   (1) 0 Γ (A) Γ(A) = 0 Γ(2) (A) This is written as: Γ = Γ(1) ⊕ Γ(2) . If this is not possible the representation is called irreducible. The number of irreducible representations equals the number of conjugacy classes.

13.2 The fundamental orthogonality theorem 13.2.1 Schur’s lemma Lemma: Each matrix which commutes with all matrices of an irreducible representation is a constant ×II, where II is the unit matrix. The opposite is (of course) also true. Lemma: If there exists a matrix M so that for two irreducible representations of group G, γ (1) (Ai ) and γ (2) (Ai ), holds: M γ (1) (Ai ) = γ (2) (Ai )M , than the representations are equivalent, or M = 0.

13.2.2 The fundamental orthogonality theorem For a set of unequivalent, irreducible, unitary representations holds that, if h is the number of elements in the group and `i is the dimension of the ith ¯ representation: X R∈G

(j)

Γ(i)∗ µν (R)Γαβ (R) =

h δij δµα δνβ `i

13.2.3 Character The character of a representation is given by the trace of the matrix and is therefore invariant for base transformations: χ(j) (R) = Tr(Γ(j) (R)) Also holds, with Nk the number of elements in a conjugacy class:

X k

Theorem:

n X i=1

`2i = h

χ(i)∗ (Ck )χ(j) (Ck )Nk = hδij

Chapter 13: Theory of groups

73

13.3 The relation with quantum mechanics 13.3.1 Representations, energy levels and degeneracy Consider a set of symmetry transformations ~x 0 = R~x which leave the Hamiltonian H invariant. These transformations are a group. An isomorfic operation on the wavefunction is given by: PR ψ(~x ) = ψ(R−1 ~x ). This is considered an active rotation. These operators commute with H: PR H = HPR , and leave the volume element unchanged: d(R~x ) = d~x. PR is the symmetry group of the physical system. It causes degeneracy: if ψn is a solution of Hψn = En ψn than also holds: H(PR ψn ) = En (PR ψn ). A degeneracy which is not the result of a symmetry is called an accidental degeneracy. (n)

Assume an `n -fold degeneracy at En : then choose an orthonormal set ψν , ν = 1, 2, . . . , `n . The function `n X (n) ψκ(n) Γ(n) PR ψν is in the same subspace: PR ψν(n) = κν (R) κ=1

where Γ is an irreducible, unitary representation of the symmetry group G of the system. Each n corresponds with another energy level. One can purely mathematical derive irreducible representations of a symmetry group and label the energy levels with a quantum number this way. A fixed choice of Γ(n) (R) defines (n) the base functions ψν . This way one can also label each separate base function with a quantum number. (n)

Particle in a periodical potential: the symmetry operation is a cyclic group: note the operator describing one translation over one unit as A. Then: G = {A, A2 , A3 , . . . , Ah = E}. The group is Abelian so all irreducible representations are one-dimensional. For 0 ≤ p ≤ h − 1 follows: Γ(p) (An ) = e2πipn/h

  2πp 2π If one defines: k = − mod , so: PA ψp (x) = ψp (x − a) = e2πip/h ψp (x), this gives Bloch’s ah a theorem: ψk (x) = uk (x)eikx , with uk (x ± a) = uk (x).

13.3.2 Breaking of degeneracy by a perturbation Suppose the unperturbed system has Hamiltonian H0 and symmetry group G0 . The perturbed system has H = H0 + V, and symmetry group G ⊂ G0 . If Γ(n) (R) is an irreducible representation of G0 , it is also a representation of G but not all elements of Γ(n) in G0 are also in G. The representation then usually becomes reducible: Γ(n) = Γ(n1 ) ⊕ Γ(n2 ) ⊕ . . .. The degeneracy is then (possibly partially) removed: see the figure below. `n1 = dim(Γ(n1 ) ) `n2 = dim(Γ(n2 ) )

`n

`n3 = dim(Γ(n3 ) ) Spectrum H

Spectrum H0

(n)

Theorem: The set of `n degenerated eigenfunctions ψν irreducible representation Γ(n) of the symmetry group.

with energy En is a basis for an `n -dimensional

13.3.3 The construction of a base function Each function F in configuration space can be decomposed into symmetry types: F =

`j n X X j=1 κ=1

The following operator extracts the symmetry types: `j X (j)∗ Γκκ (R)PR h R∈G

! F = fκ(j)

fκ(j)

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(j) (j) This is expressed as: fκ is the part of F that transforms according to the κth ¯ row of Γ . P (aj) (j) cajκ ϕκ . The functions fκ are in general not F can also be expressed in base functions ϕ: F = ajκ

transformed into each other by elements of the group. However, this does happen if cjaκ = cja . Theorem: Two wavefunctions transforming according to non-equivalent unitary representations or according to different rows of an unitary irreducible representation are orthogonal: (i) (j) (i) (i) hϕκ |ψλ i ∼ δij δκλ , and hϕκ |ψκ i is independent of κ.

13.3.4 The direct product of representations Consider a physical system existing of two subsystems. The subspace D (i) of the system transforms according (i) (1) (2) to Γ(i) . Basefunctions are ϕκ (~xi ), 1 ≤ κ ≤ `i . Now form all `1 × `2 products ϕκ (~x1 )ϕλ (~x2 ). These define a space D(1) ⊗ D(2) . These product functions transform as: (2)

(2)

x1 )ϕλ (~x2 )) = (PR ϕ(1) x1 ))(PR ϕλ (~x2 )) PR (ϕ(1) κ (~ κ (~ In general the space D(1) ⊗ D(2) can be split up in a number of invariant subspaces: X ni Γ(i) Γ(1) ⊗ Γ(2) = i

A useful tool for this reduction is that for the characters hold: X ni χ(i) (R) χ(1) (R)χ(2) (R) = i

13.3.5 Clebsch-Gordan coefficients (i)

(j)

(aκ)

With the reduction of the direct-product matrix w.r.t. the basis ϕκ ϕλ one uses a new basis ϕµ functions lie in subspaces D(ak) . The unitary base transformation is given by: X (j) = ϕ(i) ϕ(ak) µ κ ϕλ (iκjλ|akµ)

. These base

κλ (j)

and the inverse transformation by: ϕ(i) κ ϕλ =

X

ϕ(aκ) (akµ|iκjλ) µ

akµ (i)

(j)

(ak)

In essence the Clebsch-Gordan coefficients are dot products: (iκjλ|akµ) := hϕk ϕλ |ϕµ

i

13.3.6 Symmetric transformations of operators, irreducible tensor operators Observables (operators) transform as follows under symmetry transformations: A0 = PR APR−1 . If a set of (j) operators Aκ with 0 ≤ κ ≤ `j transform into each other under the transformations of G holds: −1 PR A(j) κ PR =

X

(j) A(j) ν Γνκ (R)

ν (j)

If Γ(j) is irreducible they are called irreducible tensor operators A(j) with components Aκ . P (j) ak , with: An operator can also be decomposed into symmetry types: A = jk

a(j) κ

=

! `j X (j)∗ Γκκ (R) (PR APR−1 ) h R∈G

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75

Theorem: Matrix elements Hij of the operator H which is invariant under ∀A∈G , are 0 between states which transform according to non-equivalent irreducible unitary representations or according to different rows of such (i) (i) a representation. Further hϕκ |H|ψκ i is independent of κ. For H = 1 this becomes the previous theorem. This is applied in quantum mechanics in perturbation theory and variational calculus. Here one tries to diag(i) onalize H. Solutions can be found within each category of functions ϕκ with common i and κ: H is already diagonal in categories as a whole. Perturbation calculus can be applied independent within each category. With variational calculus the try function can be chosen within a separate category because the exact eigenfunctions transform according to a row of an irreducible representation.

13.3.7 The Wigner-Eckart theorem (i)

(j)

(k)

Theorem: The matrix element hϕλ |Aκ |ψµ i can only be 6= 0 if Γ(j) ⊗ Γ(k) = . . . ⊕ Γ(i) ⊕ . . .. If this is the case holds (if Γ(i) appears only once, otherwise one has to sum over a): (i)

(k) (i) (j) (k) hϕλ |A(j) i κ |ψµ i = (iλ|jκkµ)hϕ kA kψ

This theorem can be used to determine selection rules: the probability of a dipole transition is given by (~ is the direction of polarization of the radiation): PD =

8π 2 e2 f 3 |r12 |2 with r12 = hl2 m2 |~ · ~r |l1 m1 i 3¯ hε0 c3

Further it can be used to determine intensity ratios: if there is only one value of a the ratio of the matrix elements are the Clebsch-Gordan coefficients. For more a-values relations between the intensity ratios can be stated. However, the intensity ratios are also dependent on the occupation of the atomic energy levels.

13.4 Continuous groups Continuous groups have h = ∞. However, not all groups with h = ∞ are continuous, e.g. the translation group of an spatially infinite periodic potential is not continuous but does have h = ∞.

13.4.1 The 3-dimensional translation group For the translation of wavefunctions over a distance a holds: Pa ψ(x) = ψ(x − a). Taylor expansion near x gives: dψ(x) 1 2 d2 ψ(x) + a − +... ψ(x − a) = ψ(x) − a dx 2 dx2 ¯h ∂ , this can be written as: Because the momentum operator in quantum mechanics is given by: px = i ∂x ψ(x − a) = e−iapx /¯h ψ(x)

13.4.2 The 3-dimensional rotation group This group is called SO(3) because a faithful representation can be constructed from orthogonal 3 × 3 matrices with a determinant of +1. For an infinitesimal rotation around the x-axis holds: Pδθx ψ(x, y, z) ≈ = =

ψ(x, y + zδθx , z − yδθx )   ∂ ∂ − yδθx ψ(x, y, z) ψ(x, y, z) + zδθx ∂y ∂z   iδθx Lx ψ(x, y, z) 1− ¯h

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Because the angular momentum operator is given by: Lx = So in an arbitrary direction holds:

Rotations: Translations:

¯ h i

  ∂ ∂ −y z . ∂y ∂z

Pα,~n = exp(−iα(~n · J~ )/¯h) Pa,~n = exp(−ia(~n · p~ )/¯h)

Jx , Jy and Jz are called the generators of the 3-dim. rotation group, px , py and pz are called the generators of the 3-dim. translation group. The commutation rules for the generators can be derived from the properties of the group for multiplications: translations are interchangeable ↔ px py − py px = 0. Rotations are not generally interchangeable: consider a rotation around axis ~n in the xz-plane over an angle α. Then holds: Pα,~n = P−θ,y Pα,x Pθ,y , so: ~

e−iα(~n·J )/¯h = eiθJy /¯h e−iαJx /¯h e−iθJy /¯h If α and θ are very small and are expanded to second order, and the corresponding terms are put equal with ~n · J~ = Jx cos θ + Jz sin θ, it follows from the αθ term: Jx Jy − Jy Jx = i¯hJz .

13.4.3 Properties of continuous groups The elements R(p1 , ..., pn ) depend continuously on parameters p1 , ..., pn . For the translation group this are e.g. anx , any and anz . It is demanded that the multiplication and inverse of an element R depend continuously on the parameters of R. The statement that each element arises only once in each row and column of the Cayley table holds also for continuous groups. The notion conjugacy class for continuous groups is defined equally as for discrete groups. The notion representation is fitted by demanding continuity: each matrix element depends continuously on pi (R). Summation over all group elements is for continuous groups replaced by an integration. If f (R) is a function defined on G, e.g. Γαβ (R), holds: Z Z Z f (R)dR := · · · f (R(p1 , ..., pn ))g(R(p1 , ..., pn ))dp1 · · · dpn G

p1

pn

Here, g(R) is the density function.

R R Because of the properties of the Cayley table is demanded: f (R)dR = f (SR)dR. This fixes g(R) except for a constant factor. Define new variables p0 by: SR(pi ) = R(p0i ). If one writes: dV := dp1 · · · dpn holds: g(S) = g(E)

dV dV Here, is the Jacobian: = det dV 0 dV 0

∂pi ∂p0j

!

dV dV 0

, and g(E) is constant.

For the translation group holds: g(~a) = constant = g(~0 ) because g(a~n )d~a0 = g(~0 )d~a and d~a0 = d~a. This leads to the fundamental orthogonality theorem: Z Z 1 (j) Γ(i)∗ (R)Γ (R)dR = δ δ δ dR ij µα νβ µν αβ `i G

and for the characters hold:

G

Z

Z χ(i)∗ (R)χ(j) (R)dR = δij G

Compact groups are groups with a finite group volume:

R G

dR G

dR < ∞.

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77

13.5 The group SO(3) One can take 2 parameters for the direction of the rotational axis and one for the angle of rotation ϕ. The parameter space is a collection points ϕ~n within a sphere with radius π. The diametrical points on this sphere are equivalent because R~n,π = R~n,−π . Another way to define parameters is by means of Eulers angles. If α, β and γ are the 3 Euler angles, defined as: 1. The spherical angles of axis 3 w.r.t. xyz are θ, ϕ := β, α. Now a rotation around axis 3 remains possible. 2. The spherical angles of the z-axis w.r.t. 123 are θ, ϕ := β, π − γ. then the rotation of a quantum mechanical system is described by: ~ ψ → e−iαJz h¯ e−iβJy /¯h e−iγJz /¯h ψ. So PR = e−iε(~n·J )/¯h . All irreducible representations of SO(3) can be constructed from the behaviour of the spherical harmonics Ylm (θ, ϕ) with −l ≤ m ≤ l and for a fixed l: X (l) Ylm0 (θ, ϕ)Dmm0 (R) PR Ylm (θ, ϕ) = m0

D(l) is an irreducible representation of dimension 2l + 1. The character of D (l) is given by: χ(l) (α) =

l X

eimα = 1 + 2

m=−l

l X

cos(kα) =

k=0

sin([l + 12 ]α) sin( 12 α)

In the performed derivation α is the rotational angle around the z-axis. This expression is valid for all rotations over an angle α because the classes of SO(3) are rotations around the same angle around an axis with an arbitrary orientation. Via the fundamental orthogonality theorem for characters one obtains the following expression for the density function (which is normalized so that g(0) = 1): g(α) =

sin2 ( 12 α) ( 12 α)2

With this result one can see that the given representations of SO(3) are the only ones: the character of another representation χ0 would have to be ⊥ to the already found ones, so χ0 (α) sin2 ( 12 α) = 0∀α ⇒ χ0 (α) = 0∀α. This is contradictory because the dimension of the representation is given by χ0 (0). Because fermions have an half-odd integer spin the states ψsms with s = 12 and ms = ± 21 constitute a 2-dim. space which is invariant under rotations. A problem arises for rotations over 2π: ψ 12 ms → e−2πiSz /¯h ψ 12 ms = e−2πims ψ 12 ms = −ψ 12 ms However, in SO(3) holds: Rz,2π = E. So here holds E → ±II. Because observable quantities can always be written as hφ|ψi or hφ|A|ψi, and are bilinear in the states, they do not change sign if the states do. If only one state changes sign the observable quantities do change. The existence of these half-odd integer representations is connected with the topological properties of SO(3): the group is two-fold coherent through the identification R0 = R2π = E.

13.6 Applications to quantum mechanics 13.6.1 Vectormodel for the addition of angular momentum If two subsystems have angular momentum quantum numbers j1 and j2 the only possible values for the total angular momentum are J = Pj1 + j2 , j1 + j2 − 1, ..., |j1 − j2 |. This can be derived from group theory as follows: from χ(j1 ) (α)χ(j2 ) (α) = nj χ(J) (α) follows: J

D(j1 ) ⊗ D(j2 ) = D(j1 +j2 ) ⊕ D(j1 +j2 −1) ⊕ ... ⊕ D(|j1 −j2 |)

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The states can be characterized by quantum numbers in two ways: with j1 , m1 , j2 , m2 and with j1 , j2 , J, M . The Clebsch-Gordan coefficients, for SO(3) called the Wigner coefficients, can be chosen real, so: P = ψj1 m1 j2 m2 (j1 m1 j2 m2 |JM ) ψj1 j2 JM m 1 m2 P ψj1 j2 JM (j1 m1 j2 m2 |JM ) ψj1 m1 j2 m2 = JM

13.6.2 Irreducible tensor operators, matrixelements and selection rules Some examples of the behaviour of operators under SO(3) 1. Suppose j = 0: this gives the identical representation with `j = 1. This state is described by a (0) (0) scalar operator. Because PR A0 PR−1 = A0 this operator is invariant, e.g. the Hamiltonian of a 0 0 free atom. Then holds: hJ M |H|JM i ∼ δMM 0 δJJ 0 . ~ = (Ax , Ay , Az ). The cartesian components of a vector operator transform equally 2. A vector operator: A as the cartesian components of ~r by definition. So for rotations around the z-axis holds:   cos α − sin α 0 D(Rα,z ) =  sin α cos α 0  0 0 1 operator  has the same matrix elements w.r.t. PR ψ and PR φ:

The transformed PR ψ|PR Ax PR−1 |PR φ = hψ|Ax |φi, and χ(Rα,z ) = 1 + 2 cos(α). According to the equation for characters this means one can choose base operators which transform like Y1m (θ, ϕ). These turn out to be the spherical components: 1 1 (1) (1) (1) A+1 = − √ (Ax + iAy ), A0 = Az , A−1 = √ (Ax − iAy ) 2 2 ~ and 3. A cartesian tensor of rank 2: Tij is a quantity which transforms under rotations like Ui Vj , where U P −1 = Tkl Dki (R)Dlj (R), so like D(1) ⊗ D(1) = V~ are vectors. So Tij transforms like PR Tij P R

kl

D(2) ⊕ D(1) ⊕ D(0) . The 9 components can be split in 3 invariant subspaces with dimension 1 (D (0) ), 3 (D(1) ) and 5 (D(2) ). The new base operators are: ~ ·V ~ , so as D(0) . I. Tr(T ) = Txx + Tyy + Tzz . This transforms as the scalar U ~ × V~ , II. The 3 antisymmetric components Az = 12 (Txy − Tyx ), etc. These transform as the vector U (1) so as D . III. The 5 independent components of the traceless, symmetric tensor S: Sij = 12 (Tij + Tji ) − 13 δij Tr(T ). These transform as D(2) . Selection rules for dipole transitions ~ + Dipole operators transform as D(1) : for an electric dipole transfer is the operator e~r, for a magnetic e(L ~ 2S )/2m. 0

From the Wigner-Eckart theorem follows: hJ 0 M 0 |Aκ |JM i = 0 except D(J ) is a part of D(1) ⊗ D(J) = D(J+1) ⊕ D(J) ⊕ D(|J−1|) . This means that J 0 ∈ {J + 1, J, |J − 1|}: J 0 = J or J 0 = J ± 1, except J 0 = J = 0. (1)

Land´e-equation for the anomalous Zeeman splitting According to Land´e’s model the interaction between a magnetic moment with an external magnetic field is ~ on J~ because L ~ and S ~ precede fast around J. ~ This can also be understood determined by the projection of M

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79

from the Wigner-Eckart theorem: from this follows that the matrix elements from all vector operators show a ~ follows: certain proportionality. For an arbitrary operator A ~ · J~ |αjmi hαjm|A ~ = hαjm0 |J~ |αjmi hαjm0 |A|αjmi j(j + 1)¯ h2

13.7 Applications to particle physics The physics of a system does not change after performing a transformation ψ 0 = eiδ ψ where δ is a constant. This is a global gauge transformation: the phase of the wavefunction changes everywhere by the same amount. ~ and φ at the same E ~ and B: ~ gauge transformations There exists some freedom in the choice of the potentials A ~ and B ~ (See chapter 2 and 10). The solution ψ 0 of the Schr¨odinger equation of the potentials do not change E with the transformed potentials is: ψ 0 = e−iqf (~r,t) ψ. This is a local gauge transformation: the phase of the wavefunction changes different at each position. The ~ and φ are also transformed. This is now stated as a guide principle: physics of the system does not change if A the “right of existence” of the electromagnetic field is to allow local gauge invariance. The gauge transformations of the EM-field form a group: U(1), unitary 1 × 1-matrices. The split-off of charge in the exponent is essential: it allows one gauge field for all charged particles, independent of their charge. This concept is generalized: particles have a “special charge” Q. The group elements now are PR = exp(−iQΘ). Other force fields than the electromagnetic field can also be understood this way. The weak interaction together with the electromagnetic interaction can be described by a force field that transforms according to U(1)⊗SU(2), and consists of the photon and three intermediary vector bosons. The colour force is described by SU(3), and has a gauge field that exists of 8 types of gluons. ~ where Θn are real constants and Tn operators In general the group elements are given by PR = exp(−iT~ · Θ), P (generators), like Q. The commutation rules are given by [Ti , Tj ] = i cijk Tk . The cijk are the structure k

constants of the group. For SO(3) these constants are cijk = εijk , here εijk is the complete antisymmetric tensor with ε123 = +1. These constants can be found with the help of group product elements: because G is closed holds: ~ ~ ~0 ~ ~ ~ ~0 ~ ~ 00 ~ eiΘ·T eiΘ ·T e−iΘ·T e−iΘ ·T = e−iΘ ·T . Taylor expansion and setting equal Θn Θ0m -terms results in the commutation rules. The group SU(2) has 3 free parameters: because it is unitary there are 4 real conditions over 4 complex parameters, and the determinant has to be +1, remaining 3 free parameters. Each unitary matrix U can be written as: U = e−iH . Here, H is a Hermitian matrix. Further it always holds that: det(U ) = e−iTr(H) . For each matrix of SU(2) holds that Tr(H)=0. Each Hermitian, traceless 2 × 2 matrix can be written as a linear combination of the 3 Pauli-matrices σi . So these matrices are a choice for the operators of SU(2). One can ~ write: SU(2)={exp(− 1 i~σ · Θ)}. 2

In abstraction, one can consider an isomorphic group where only the commutation rules are considered to be known regarding the operators Ti : [T1 , T2 ] = iT3 , etc. In elementary particle physics the Ti can be interpreted e.g. as the isospin operators. Elementary particles can be classified in isospin-multiplets, these are the irreducible representations of SU(2). The classification is: ~ ~

1. The isospin-singlet ≡ the identical representation: e−iT ·Θ = 1 ⇒ Ti = 0 2. The isospin-doublet ≡ the faithful representation of SU(2) on 2 × 2 matrices.

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The group SU(3) has 8 free parameters. (The group SU(N ) has N 2 − 1 free parameters). The Hermitian, traceless operators are 3 SU(2)-subgroups in the ~e1~e2 , ~e1~e3 and the ~e2~e3 plane. This gives 9 matrices, which are not all 9 linear independent. By taking a linear combination one gets 8 matrices. X D ∂ ∂ → := − Ti Aix ∂x Dx ∂x i=1 8

In the Lagrange density for the colour force one has to substitute

The terms of 3rd and 4th power in A show that the colour field interacts with itself.

Chapter 14

Nuclear physics 14.1 Nuclear forces The mass of a nucleus is given by: Mnucl = Zmp + N mn − Ebind /c2 The binding energy per nucleon is given in the figure at the right. The top is at 56 26 Fe, the most stable nucleus. With the constants a1 a2 a3 a4 a5

= = = = =

15.760 17.810 0.711 23.702 34.000

MeV MeV MeV MeV MeV

9 8 ↑ 7 E 6 (MeV) 5 4 3 2 1 0

0

40

80

120 160 A→

200

240

and A = Z + N , in the droplet or collective model of the nucleus the binding energy Ebind is given by: Z(Z − 1) (N − Z)2 Ebind + a5 A−3/4 = a1 A − a2 A2/3 − a3 − a4 2 1/3 c A A These terms arise from: 1. a1 : Binding energy of the strong nuclear force, approximately ∼ A. 2. a2 : Surface correction: the nucleons near the surface are less bound. 3. a3 : Coulomb repulsion between the protons. 4. a4 : Asymmetry term: a surplus of protons or neutrons has a lower binding energy. 5. a5 : Pair off effect: nuclei with an even number of protons or neutrons are more stable because groups of two protons or neutrons have a lower energy. The following holds: Z even, N even:  = +1, Z odd, N odd:  = −1. Z even, N odd:  = 0, Z odd, N even:  = 0. The Yukawa potential can be derived if the nuclear force can to first approximation, be considered as an exchange of virtual pions:   r W0 r0 exp − U (r) = − r r0 ¯ /m0 c. With ∆E · ∆t ≈ ¯ h, Eγ = m0 c2 and r0 = c∆t follows: r0 = h In the shell model of the nucleus one assumes that a nucleon moves in an average field of other nucleons. ~ · S: ~ ∆Vls = 1 (2l + 1)¯hω. So each level Further, there is a contribution of the spin-orbit coupling ∼ L 2 1 (n, l) is split in two, with j = l ± 2 , where the state with j = l + 12 has the lowest energy. This is just the opposite for electrons, which is an indication that the L − S interaction is not electromagnetical. The energy of a 3-dimensional harmonic oscillator is E = (N + 32 )¯hω. N = nx + ny + nz = 2(n − 1) + l where n ≥ 1 is the main oscillator number. Because −l ≤ m ≤ l and ms = ± 12 ¯h there are 2(2l + 1) 81

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82

substates which exist independently for protons and neutrons. This gives rise to the so called magical numbers: nuclei where each state in the outermost level are filled are particulary stable. This is the case if N or Z ∈ {2, 8, 20, 28, 50, 82, 126}.

14.2 The shape of the nucleus A nucleus is to first approximation spherical with a radius of R = R0 A1/3 . Here, R0 ≈ 1.4·10−15 m, constant for all nuclei. If the nuclear radius is measured including the charge distribution one obtains R0 ≈ 1.2 · 10−15 m. The shape of oscillating nuclei can be described by spherical harmonics: # " X m alm Yl (θ, ϕ) R = R0 1 + lm

l = 0 gives rise to monopole vibrations, density vibrations, which can be applied to the √ theory of neutron stars. l = 1 gives dipole vibrations, l = 2 quadrupole, with a2,0 = β cos γ and a2,±2 = 12 2β sin γ where β is the deformation factor and γ the shape parameter. The multipole moment is given by µl = Zerl Ylm (θ, ϕ). The parity of the electric moment is ΠE = (−1)l , of the magnetic moment ΠM = (−1)l+1 . ~ and M ~ S = gS e S. ~ ~L = e L There are 2 contributions to the magnetic moment: M 2mp 2mp where gS is the spin-gyromagnetic ratio. For protons holds gS = 5.5855 and for neutrons gS = −3.8263. The z-components of the magnetic moment are given by ML,z = µN ml and MS,z = gS µN mS . The resulting ~ The z-component is then ~ = gI (e/2mp)I. magnetic moment is related to the nuclear spin I according to M Mz = µN gI mI .

14.3 Radioactive decay The number of nuclei decaying is proportional to the number of nuclei: N˙ = −λN . This gives for the number of nuclei N : N (t) = N0 exp(−λt). The half life time follows from τ 12 λ = ln(2). The average life time of a nucleus is τ = 1/λ. The probability that N nuclei decay within a time interval is given by a Poisson distribution: λN e−λ dt P (N )dt = N0 N! P If a P nucleus can decay into more final states then holds: λ = λi . So the fraction decaying into state i is λi / λi . There are 5 types of natural radioactive decay: 1. α-decay: the nucleus emits a He2+ nucleus. Because nucleons tend to order themselves in groups of 2p+2n this can be considered as a tunneling of a He2+ nucleus through a potential barrier. The tunnel probability P is s Z 1 incoming amplitude −2G =e with G = 2m [V (r) − E]dr P = outgoing amplitude ¯h G is called the Gamow factor. 2. β-decay. Here a proton changes into a neutron or vice versa: p+ → n0 + W+ → n0 + e+ + νe , and n0 → p+ + W− → p+ + e− + ν e . 3. Electron capture: here, a proton in the nucleus captures an electron (usually from the K-shell). 4. Spontaneous fission: a nucleus breaks apart. 5. γ-decay: here the nucleus emits a high-energetic photon. The decay constant is given by 2l  Eγ Eγ R P (l) ∼ ∼ 10−4l λ= ¯hω (¯hc)2 ¯hc

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83

where l is the quantum number for the angular momentum and P the radiated power. Usually the decay constant of electric multipole moments is larger than the one of magnetic multipole moments. The energy of the photon is Eγ = Ei − Ef − TR , with TR = Eγ2 /2mc2 the recoil energy, which can usually be neglected. The parity of the emitted radiation is Πl = Πi · Πf . With I the quantum p number of angular momentum of the nucleus, L = h ¯ I(I + 1), holds the following selection rule: |I~i − I~f | ≤ ∆l ≤ |I~i + I~f |.

14.4 Scattering and nuclear reactions 14.4.1 Kinetic model If a beam with intensity I hits a target with density n and length x (Rutherford scattering) the number of scatterings R per unit of time is equal to R = Inxσ. From this follows that the intensity of the beam decreases as −dI = Inσdx. This results in I = I0 e−nσx = I0 e−µx . Because dR = R(θ, ϕ)dΩ/4π = Inxdσ it follows:

R(θ, ϕ) dσ = dΩ 4πnxI

If N particles are scattered in a material with density n then holds: Z1 Z2 e2 1 dσ = For Coulomb collisions holds: 2 4 dΩ C 8πε0 µv0 sin ( 12 θ)

dσ ∆N = n ∆Ω∆x N dΩ

14.4.2 Quantum mechanical model for n-p scattering The initial state is a beam of neutrons moving along the z-axis with wavefunction ψinit = eikz and current density Jinit = v|ψinit |2 = v. At large distances from the scattering point they have approximately a spherical wavefunction ψscat = f (θ)eikr /r where f (θ) is the scattering amplitude. The total wavefunction is then given by eikr ψ = ψin + ψscat = eikz + f (θ) r The particle flux of the scattered particles is v|ψscat |2 = v|f (θ)|2 dΩ. From this it follows that σ(θ) = |f (θ)|2 . The wavefunction of the incoming particles can be expressed as a sum of angular momentum wavefunctions: ψinit = eikz =

X

ψl

l

The impact parameter is related to the angular momentum with L = bp = b¯hk, so bk ≈ l. At very low energy only particles with l = 0 are scattered, so ψ = ψ00 +

X

ψl and ψ0 =

l>0

If the potential is approximately rectangular holds: ψ00 = C The cross section is then σ(θ) =

sin2 (δ0 ) so σ = k2

At very low energies holds: sin2 (δ0 ) =

Z

sin(kr) kr

sin(kr + δ0 ) kr

σ(θ)dΩ =

4π sin2 (δ0 ) k2

¯ 2 k 2 /2m h W0 + W

with W0 the depth of the potential well. At higher energies holds: σ =

4π X 2 sin (δl ) k2 l

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14.4.3 Conservation of energy and momentum in nuclear reactions If a particle P1 collides with a particle P2 which is in rest w.r.t. the laboratory system and other particles are created, so X Pk P1 + P2 → k>2

the total energy Q gained or required is given by Q = (m1 + m2 −

P

mk )c2 .

k>2

The minimal required kinetic energy T of P1 in the laboratory system to initialize the reaction is P m1 + m2 + mk T = −Q 2m2 If Q < 0 there is a threshold energy.

14.5 Radiation dosimetry Radiometric quantities determine the strength of the radiation source(s). Dosimetric quantities are related to the energy transfer from radiation to matter. Parameters describing a relation between those are called interaction parameters. The intensity of a beam of particles in matter decreases according to I(s) = I0 exp(−µs). The deceleration of a heavy particle is described by the Bethe-Bloch equation: q2 dE ∼ 2 ds v The fluention is given by Φ = dN/dA. The flux is given by φ = dΦ/dt. The energy loss is defined by Ψ = dW/dA, and the energy flux density ψ = dΨ/dt. The absorption coefficient is given by µ = (dN/N )/dx. The mass absorption coefficient is given by µ/%. The radiation dose X is the amount of charge produced by the radiation per unit of mass, with unit C/kg. An old unit is the R¨ontgen: 1Ro= 2.58 · 10−4 C/kg. With the energy-absorption coefficient µE follows: X=

eµE dQ = Ψ dm W%

where W is the energy required to disjoin an elementary charge. The absorbed dose D is given by D = dEabs /dm, with unit Gy=J/kg. An old unit is the rad: 1 rad=0.01 Gy. ˙ It can be derived that The dose tempo is defined as D. D=

µE Ψ %

The Kerma K is the amount of kinetic energy of secundary produced particles which is produced per mass unit of the radiated object. The equivalent dose H is a weight average of the absorbed dose per type of radiation, where for each type radiation the effects on biological material is used for the weight factor. These weight factors are called the quality factors. Their unit is Sv. P H = QD. If the absorption is not equally distributed also weight factors w per organ need to be used: H = wk Hk . For some types of radiation holds: Radiation type R¨ontgen, gamma radiation β, electrons, mesons Thermic neutrons Fast neutrons protons α, fission products

Q 1 1 3 to 5 10 to 20 10 20

Chapter 15

Quantum field theory & Particle physics 15.1 Creation and annihilation operators A state with more particles can be described by a collection occupation numbers |n1 n2 n3 · · ·i. Hence the vacuum state is given by |000 · · ·i. This is a complete description because the particles are indistinguishable. The states are orthonormal: ∞ Y δni n0i hn1 n2 n3 · · · |n01 n02 n03 · · ·i = i=1

The time-dependent state vector is given by X

Ψ(t) =

cn1 n2 ··· (t)|n1 n2 · · ·i

n1 n2 ···

The coefficients c can be interpreted as follows: |cn1 n2 ··· |2 is the probability to find n1 particles with momenP tum ~k1 , n2 particles with momentum ~k2 , etc., and hΨ(t)|Ψ(t)i = |cni (t)|2 = 1. The expansion of the states in time is described by the Schr¨odinger equation i

d |Ψ(t)i = H|Ψ(t)i dt

where H = H0 + Hint . H0 is the Hamiltonian for free particles and keeps |cni (t)|2 constant, Hint is the interaction Hamiltonian and can increase or decrease a c2 at the cost of others. All operators which can change occupation numbers can be expanded in the a and a† operators. a is the annihilation operator and a† the creation operator, and: √ ni |n1 n2 · · · ni − 1 · · ·i a(~ki )|n1 n2 · · · ni · · ·i = √ † ~ ni + 1 |n1 n2 · · · ni + 1 · · ·i a (ki )|n1 n2 · · · ni · · ·i = Because the states are normalized holds a|0i = 0 and a(~ki )a† (~ki )|ni i = ni |ni i. So aa† is an occupation number operator. The following commutation rules can be derived: [a(~ki ), a(~kj )] = 0 , [a† (~ki ), a† (~kj )] = 0 , [a(~ki ), a† (~kj )] = δij P †~ Hence for free spin-0 particles holds: H0 = a (ki )a(~ki )¯hωki i

15.2 Classical and quantum fields Starting with a real field Φα (x) (complex fields can be split in a real and an imaginary part), the Lagrange density L is a function of Rthe position x = (~x, ict) through the fields: L = L(Φα (x), ∂ν Φα (x)). The LagrangianRis given by L = L(x)d3 x. Using the variational principle δI(Ω) = 0 and with the action-integral I(Ω) = L(Φα , ∂ν Φα )d4 x the field equation can be derived: ∂ ∂L ∂L =0 − α ∂Φ ∂xν ∂(∂ν Φα ) The conjugated field is, analogous to momentum in classical mechanics, defined as: Πα (x) =

85

∂L ˙α ∂Φ

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˙ α − L(x). With this, the Hamilton density becomes H(x) = Πα Φ Quantization of a classical field is analogous to quantization in point mass mechanics: the field functions are considered as operators obeying certain commutation rules: [Φα (~x), Φβ (~x 0 )] = 0 , [Πα (~x), Πβ (~x 0 )] = 0 , [Φα (~x), Πβ (~x 0 )] = iδαβ (~x − ~x 0 )

15.3 The interaction picture Some equivalent formulations of quantum mechanics are possible: 1. Schr¨odinger picture: time-dependent states, time-independent operators. 2. Heisenberg picture: time-independent states, time-dependent operators. 3. Interaction picture: time-dependent states, time-dependent operators. The interaction picture can be obtained from the Schr¨odinger picture by an unitary transformation: S

S

S

|Φ(t)i = eiH0 |ΦS (t)i and O(t) = eiH0 OS e−iH0 The index S denotes the Schr¨odinger picture. From this follows: i

d d |Φ(t)i = Hint (t)|Φ(t)i and i O(t) = [O(t), H0 ] dt dt

15.4 Real scalar field in the interaction picture It is easy to find that, with M := m20 c2 /¯ h2 , holds: ∂ ∂ Φ(x) = Π(x) and Π(x) = (∇2 − M 2 )Φ(x) ∂t ∂t From this follows that Φ obeys the Klein-Gordon equation (2 − M 2 )Φ = 0. With the definition k02 = ~k 2 + M 2 := ω 2 and the notation ~k · ~x − ik0 t := kx the general solution of this equation is: k q   X i X 1  1  ~ ikx 1 ~ ikx + a† (~k )e−ikx √ a(k )e + a† (~k )e−ikx , Π(x) = √ Φ(x) = √ 2 ωk −a(k )e 2ωk V ~ V ~ k

k

The field operators contain a volume V , which is used as normalization factor. Usually one can take the limit V → ∞. In general it holds that the term with e−ikx , the positive frequency part, is the creation part, and the negative frequency part is the annihilation part. the coefficients have to be each others hermitian conjugate because Φ is hermitian. Because Φ has only one component this can be interpreted as a field describing a particle with spin zero. From this follows that the commutation rules are given by [Φ(x), Φ(x0 )] = i∆(x − x0 ) with Z 1 sin(ky) 3 d k ∆(y) = (2π)3 ωk ∆(y) is an odd function which is invariant for proper Lorentz transformations (no mirroring). This is consistent with the previously found result [Φ(~x, t, Φ(~x 0 , t)] = 0. In general holds that ∆(y) = 0 outside the light cone. So the equations obey the locality postulate. The Lagrange density is given by: L(Φ, ∂ν Φ) = − 12 (∂ν Φ∂ν Φ + m2 Φ2 ). The energy operator is given by: Z X ¯hωk a† (~k )a(~k ) H = H(x)d3 x = ~ k

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15.5 Charged spin-0 particles, conservation of charge The Lagrange density of charged spin-0 particles is given by: L = −(∂ν Φ∂ν Φ∗ + M 2 ΦΦ∗ ). Noether’s theorem connects a continuous symmetry of L and an additive conservation law. Suppose that L ((Φα )0 , ∂ν (Φα )0 ) = L (Φα , ∂ν Φα ) and there exists a continuous transformation between Φα and Φα 0 such as Φα 0 = Φα + f α (Φ). Then holds   ∂L ∂ α f =0 ∂xν ∂(∂ν Φα ) This is a continuity equation ⇒ conservation law. Which quantity is conserved depends on the symmetry. The above Lagrange density is invariant for a change in phase Φ → Φeiθ : a global gauge transformation. The conserved quantity is the current density Jµ (x) = −ie(Φ∂µ Φ∗ − Φ∗ ∂µ Φ). Because this quantity is 0 for real fields a complex field is needed to describe charged particles. When this field is quantized the field operators are given by   1 X 1  † ~ ikx 1 X 1  ~ ikx √ √ a(k )e + b† (~k )e−ikx , Φ† (x) = √ a (k )e + b(~k )e−ikx Φ(x) = √ 2ωk 2ωk V ~ V ~ k

k

Hence the energy operator is given by: H=

X

  ¯hωk a† (~k )a(~k ) + b† (~k )b(~k )

~ k

and the charge operator is given by: Z  X  e a† (~k )a(~k ) − b† (~k )b(~k ) Q(t) = −i J4 (x)d3 x ⇒ Q = ~ k

From this follows that a† a := N+ (~k ) is an occupation number operator for particles with a positive charge and b† b := N− (~k ) is an occupation number operator for particles with a negative charge.

15.6 Field functions for spin- 12 particles Spin is defined by the behaviour of the solutions ψ of the Dirac equation. A scalar field Φ has the property ˜ that, if it obeys the Klein-Gordon equation, the rotated field Φ(x) := Φ(Λ−1 x) also obeys it. Λ denotes 4-dimensional rotations: the proper Lorentz transformations. These can be written as:   ∂ ∂ ~ −i~ n ·L ˜ with Lµν = −i¯h xµ − xν Φ(x) = Φ(x)e ∂xν ∂xµ For µ ≤ 3, ν ≤ 3 these are rotations, for ν = 4, µ 6= 4 these are Lorentz transformations. ˜ A rotated field ψ˜ obeys the Dirac equation if the following condition holds: ψ(x) = D(Λ)ψ(Λ−1 x). This ~ 1 −1 i~ n ·S with Sµν = −i 2 ¯hγµ γν . Hence: results in the condition D γλ D = Λλµ γµ . One finds: D = e ˜ ψ(x) = e−i(S+L) ψ(x) = e−iJ ψ(x) Then the solutions of the Dirac equation are given by: p )e−i(~p·~x±Et) ψ(x) = ur± (~ Here, r is an indication for the direction of the spin, and ± is the sign of the energy. With the notation p ) = ur− (−~ p ) and ur (~ p ) = ur+ (~ p ) one can write for the dot products of these spinors: v r (~ 0

p )ur+ (~ p) = ur+ (~

0 0 E E δrr0 , ur− (~ δrr0 , ur+ (~ p )ur− (~ p) = p )ur− (~ p) = 0 M M

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Because of the factor E/M this is not relativistic invariant. A Lorentz-invariant dot product is defined by ab := a† γ4 b, where a := a† γ4 is a row spinor. From this follows: 0

0

0

ur (~ p )ur (~ p ) = δrr0 , v r (~ p )v r (~ p ) = −δrr0 , ur (~ p )v r (~ p) = 0 Combinations of the type aa give a 4 × 4 matrix: 2 X

u

r

(~ p )ur (~ p)

r=1

2 X −iγλ pλ + M −iγλ pλ − M , = v r (~ p )v r (~ p) = 2M 2M r=1

The Lagrange density which results in the Dirac equation and having the correct energy normalization is:   ∂ + M ψ(x) L(x) = −ψ(x) γµ ∂xµ and the current density is Jµ (x) = −ieψγµ ψ.

15.7 Quantization of spin- 12 fields The general solution for the fieldoperators is in this case: r
MX 1 X √ p )ur (~ p )eipx + d†r (~ p )v r (~ p )e−ipx cr (~ ψ(x) = V E r p ~ r

and ψ(x) =


MX 1 X † √ p )ur (~ p )e−ipx + dr (~ p )v r (~ p )eipx cr (~ V E r p ~

Here, c† and c are the creation respectively annihilation operators for an electron and d† and d the creation respectively annihilation operators for a positron. The energy operator is given by H=

X p ~

Ep~

2 X


p )cr (~ p ) − dr (~ p )d†r (~ p) c†r (~

r=1

To prevent that the energy of positrons is negative the operators must obey anti commutation rules in stead of commutation rules: p ), c†r0 (~ p )]+ = [dr (~ p ), d†r0 (~ p )]+ = δrr0 δpp0 , all other anti commutators are 0. [cr (~ The field operators obey [ψα (x), ψβ (x0 )] = 0 , [ψα (x), ψβ (x0 )] = 0 , [ψα (x), ψβ (x0 )]+ = −iSαβ (x − x0 )   ∂ − M ∆(x) with S(x) = γλ ∂xλ The anti commutation rules give besides the positive-definite energy also the Pauli exclusion principle and the p )c†r (~ p ) = −c†r (~ p )c†r (~ p ) holds: {c†r (p)}2 = 0. It appears to be impossible Fermi-Dirac statistics: because c†r (~ to create two electrons with the same momentum and spin. This is the exclusion principle. Another way to see p )}2 = Nr+ (~ p ): the occupation operators have only eigenvalues 0 and 1. this is the fact that {Nr+ (~ To avoid infinite vacuum contributions to the energy and charge the normal product is introduced. The expression for the current density now becomes Jµ = −ieN (ψγµ ψ). This product is obtained by: • Expand all fields into creation and annihilation operators, • Keep all terms which have no annihilation operators, or in which they are on the right of the creation operators, • In all other terms interchange the factors so that the annihilation operators go to the right. By an interchange of two fermion operators add a minus sign, by interchange of two boson operators not. Assume hereby that all commutators are zero.

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89

15.8 Quantization of the electromagnetic field Starting with the Lagrange density L = − 12

∂Aν ∂Aν ∂xµ ∂xµ

it follows for the field operators A(x): 4  1 X 1 X √ am (~k )m (~k )eikx + a† (~k )m (~k )∗ e−ikx A(x) = √ 2ωk m=1 V ~ k

The operators obey [am (~k ), a†m0 (~k )] = δmm0 δkk0 . All other commutators are 0. m gives the polarization direction of the photon: m = 1, 2 gives transversal polarized, m = 3 longitudinal polarized and m = 4 timelike polarized photons. Further holds: [Aµ (x), Aν (x0 )] = iδµν D(x − x0 ) with D(y) = ∆(y)|m=0 In spite of the fact that A4 = iV is imaginary in the classical case, A4 is still defined to be hermitian because otherwise the sign of the energy becomes incorrect. By changing the definition of the inner product in configuration space the expectation values for A1,2,3 (x) ∈ IR and for A4 (x) become imaginary. If the potentials satisfy the Lorentz gauge condition ∂µ Aµ = 0 the E and B operators derived from these potentials will satisfy the Maxwell equations. However, this gives problems with the commutation rules. It is now demanded that only those states are permitted for which holds ∂A+ µ |Φi = 0 ∂xµ   ∂Aµ = 0. ∂xµ

This results in:

From this follows that (a3 (~k ) − a4 (~k ))|Φi = 0. With a local gauge transformation one obtains N3 (~k ) = 0 and N4 (~k ) = 0. However, this only applies to free EM-fields: in intermediary states in interactions there can exist longitudinal and timelike photons. These photons are also responsible for the stationary Coulomb potential.

15.9 Interacting fields and the S-matrix The S(scattering)-matrix gives a relation between the initial and final states of an interaction: |Φ(∞)i = S|Φ(−∞)i. If the Schr¨odinger equation is integrated: Zt |Φ(t)i = |Φ(−∞)i − i

Hint (t1 )|Φ(t1 )idt1

−∞

and perturbation theory is applied one finds that: S=

Z Z ∞ ∞ X X (−i)n · · · T {Hint (x1 ) · · · Hint (xn )} d4 x1 · · · d4 xn ≡ S (n) n! n=0 n=0

Here, the T -operator means a time-ordered product: the terms in such a product must be ordered in increasing time order from the right to the left so that the earliest terms act first. The S-matrix is then given by: Sij = hΦi |S|Φj i = hΦi |Φ(∞)i. The interaction Hamilton density for the interaction between the electromagnetic and the electron-positron field is: Hint (x) = −Jµ (x)Aµ (x) = ieN (ψγµ ψAµ )   − When this is expanded as: Hint = ieN (ψ + + ψ − )γµ (ψ + + ψ − )(A+ µ + Aµ )

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90

eight terms appear. Each term corresponds with a possible process. The term ieψ + γµ ψ + A− µ acting on |Φi − + + gives transitions where Aµ creates a photon, ψ annihilates an electron and ψ annihilates a positron. Only terms with the correct number of particles in the initial and final state contribute to a matrix element hΦi |S|Φj i. Further the factors in Hint can create and thereafter annihilate particles: the virtual particles. The expressions for S (n) contain time-ordered products of normal products. This can be written as a sum of normal products. The appearing operators describe the minimal changes necessary to change the initial state into the final state. The effects of the virtual particles are described by the (anti)commutator functions. Some time-ordened products are: T {Φ(x)Φ(y)} o n T ψα (x)ψβ (y)

= N {Φ(x)Φ(y)} + 12 ∆F (x − y) n o F = N ψα (x)ψβ (y) − 12 Sαβ (x − y)

T {Aµ (x)Aν (y)}

F = N {Aµ (x)Aν (y)} + 12 δµν Dµν (x − y)

Here, S F (x) = (γµ ∂µ − M )∆F (x), DF (x) = ∆F (x)|m=0 and  Z ikx 1 e   d3 k  3  (2π) ω~k  ∆F (x) = Z −ikx   e 1    d3 k 3 (2π) ω~k

if x0 > 0

if x0 < 0

The term 12 ∆F (x − y) is called the contraction of Φ(x) and Φ(y), and is the expectation value of the timeordered product in the vacuum state. Wick’s theorem gives an expression for the time-ordened product of an arbitrary number of field operators. The graphical representation of these processes are called Feynman diagrams. In the x-representation each diagram describes a number of processes. The contraction functions can also be written as: Z Z −2i −2i iγµ pµ − M 4 eikx F 4 F d k and S (x) = lim d p eipx 2 ∆ (x) = lim →0 (2π)4 →0 (2π)4 k 2 + m2 − i p + M 2 − i In the expressions for S (2) this gives rise to terms δ(p + k − p0 − k 0 ). This means that energy and momentum is conserved. However, virtual particles do not obey the relation between energy and momentum.

15.10 Divergences and renormalization It turns out that higher orders contribute infinite terms because only the sum p + k of the four-momentum of the virtual particles is fixed. An integration over one of them becomes ∞. In the x-representation this can be understood because the product of two functions containing δ-like singularities is not well defined. This is solved by discounting all divergent diagrams in a renormalization of e and M . It is assumed that an electron, if there would not be an electromagnetical field, would have a mass M0 and a charge e0 unequal to the observed mass M and charge e. In the Hamilton and Lagrange density of the free electron-positron field appears M0 . So this gives, with M = M0 + ∆M : Le−p (x) = −ψ(x)(γµ ∂µ + M0 )ψ(x) = −ψ(x)(γµ ∂µ + M )ψ(x) + ∆M ψ(x)ψ(x) and Hint = ieN (ψγµ ψAµ ) − i∆eN (ψγµ ψAµ ).

15.11 Classification of elementary particles Elementary particles can be categorized as follows: 1. Hadrons: these exist of quarks and can be categorized in: I. Baryons: these exist of 3 quarks or 3 antiquarks.

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II. Mesons: these exist of one quark and one antiquark. 2. Leptons: e± , µ± , τ ± , νe , νµ , ντ , ν e , ν µ , ν τ . 3. Field quanta: γ, W± , Z0 , gluons, gravitons (?). An overview of particles and antiparticles is given in the following table: Particle u d s c b t e− µ− τ− νe νµ ντ γ gluon W+ Z graviton

spin (¯ h) B 1/2 1/3 1/2 1/3 1/2 1/3 1/2 1/3 1/2 1/3 1/2 1/3 1/2 0 1/2 0 1/2 0 1/2 0 1/2 0 1/2 0 1 0 1 0 1 0 1 0 2 0

L 0 0 0 0 0 0 1 1 1 1 1 1 0 0 0 0 0

T 1/2 1/2 0 0 0 0 0 0 0 0 0 0 0 0 0 0 0

T3 1/2 −1/2 0 0 0 0 0 0 0 0 0 0 0 0 0 0 0

S 0 0 −1 0 0 0 0 0 0 0 0 0 0 0 0 0 0

C 0 0 0 1 0 0 0 0 0 0 0 0 0 0 0 0 0

B∗ 0 0 0 0 −1 0 0 0 0 0 0 0 0 0 0 0 0

charge (e) +2/3 −1/3 −1/3 +2/3 −1/3 +2/3 −1 −1 −1 0 0 0 0 0 +1 0 0

m0 (MeV) 5 9 175 1350 4500 173000 0.511 105.658 1777.1 0(?) 0(?) 0(?) 0 0 80220 91187 0

antipart. u d s c b t e+ µ+ τ+ νe νµ ντ γ gluon W− Z graviton

Here B is the baryon number and L the lepton number. It is found that there are three different lepton numbers, one for e, µ and τ , which are separately conserved. T is the isospin, with T3 the projection of the isospin on the third axis, C the charmness, S the strangeness and B∗ the bottomness. The anti particles have quantum numbers with the opposite sign except for the total isospin T. The composition of (anti)quarks of the hadrons is given in the following table, together with their mass in MeV in their ground state: π0 π+ π− K0 K0 K+ K− D+ D− D0 D0 F+ F−

1 2

√

2(uu+dd) ud du sd ds us su cd dc cu uc cs sc

134.9764 139.56995 139.56995 497.672 497.672 493.677 493.677 1869.4 1869.4 1864.6 1864.6 1969.0 1969.0

J/Ψ Υ p+ p− n0 n0 Λ Λ Σ+ Σ− Σ0 Σ0 Σ−

cc bb uud uud udd udd uds uds uus uus uds uds dds

3096.8 9460.37 938.27231 938.27231 939.56563 939.56563 1115.684 1115.684 1189.37 1189.37 1192.55 1192.55 1197.436

Σ+ Ξ0 0 Ξ Ξ− Ξ+ Ω− Ω+ Λ+ c ∆2− ∆2+ ∆+ ∆0 ∆−

dds uss uss dss dss sss sss udc uuu uuu uud udd ddd

1197.436 1314.9 1314.9 1321.32 1321.32 1672.45 1672.45 2285.1 1232.0 1232.0 1232.0 1232.0 1232.0

Each quark can exist in two spin states. So mesons are bosons with spin 0 or 1 in their ground state, while baryons are fermions with spin 12 or 32 . There exist excited states with higher internal L. Neutrino’s have a helicity of − 21 while antineutrino’s have only + 21 as possible value. The quantum numbers are subject to conservation laws. These can be derived from symmetries in the Lagrange density: continuous symmetries give rise to additive conservation laws, discrete symmetries result in multiplicative conservation laws. Geometrical conservation laws are invariant under Lorentz transformations and the CPT-operation. These are: 1. Mass/energy because the laws of nature are invariant for translations in time.

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92

2. Momentum because the laws of nature are invariant for translations in space. 3. Angular momentum because the laws of nature are invariant for rotations. Dynamical conservation laws are invariant under the CPT-operation. These are: 1. Electrical charge because the Maxwell equations are invariant under gauge transformations. 2. Colour charge is conserved. 3. Isospin because QCD is invariant for rotations in T-space. 4. Baryon number and lepton number are conserved but not under a possible SU(5) symmetry of the laws of nature. 5. Quarks type is only conserved under the colour interaction. 6. Parity is conserved except for weak interactions. The elementary particles can be classified into three families: leptons

quarks

antileptons

antiquarks

1st generation

−

e νe

d u

+

e νe

d u

2nd generation

µ− νµ

s c

µ+ νµ

s c

3rd generation

τ− ντ

b t

τ+ ντ

b t

Quarks exist in three colours but because they are confined these colours cannot be seen directly. The color force does not decrease with distance. The potential energy will become high enough to create a quarkantiquark pair when it is tried to disjoin an (anti)quark from a hadron. This will result in two hadrons and not in free quarks.

15.12 P and CP-violation It is found that the weak interaction violates P-symmetry, and even CP-symmetry is not conserved. Some processes which violate P symmetry but conserve the combination CP are: 1. µ-decay: µ− → e− + νµ + ν e . Left-handed electrons appear more than 1000× as much as right-handed ones. 2. β-decay of spin-polarized 60 Co: 60 Co →60 Ni + e− + ν e . More electrons with a spin parallel to the Co than with a spin antiparallel are created: (parallel−antiparallel)/(total)=20%. 3. There is no connection with the neutrino: the decay of the Λ particle through: Λ → p+ + π − and Λ → n0 + π 0 has also these properties. The CP-symmetry was found to be violated by the decay of neutral Kaons. These are the lowest possible states with a s-quark so they can decay only weakly. The following holds: C|K0 i = η|K0 i where η is a phase factor. Further holds P|K0 i = −|K0 i because K0 and K0 have an intrinsic parity of −1. From this follows that K0 and K0 are not eigenvalues of CP: CP|K0 i = |K0 i. The linear combinations √ √ |K01 i := 12 2(|K0 i + |K0 i) and |K02 i := 12 2(|K0 i − |K0 i) are eigenstates of CP: CP|K01 i = +|K01 i and CP|K02 i = −|K02 i. A base of K01 and K02 is practical while describing weak interactions. For colour interactions a base of K0 and K0 is practical because then the number u−number u is constant. The expansion postulate must be used for weak decays: |K0 i = 12 (hK01 |K0 i + hK02 |K0 i)

Chapter 15: Quantum field theory & Particle physics

The probability to find a final state with CP= −1 is  1 0 0 2 | K |K . | 1 2

1 2|

93

0 0 2 K2 |K | , the probability of CP=+1 decay is

The relation between the mass eigenvalues of the quarks (unaccented) and the fields arising in the weak currents (accented) is (u0 , c0 , t0 ) = (u, c, t), and:      0  sin θ1 0 1 0 0 1 0 0 cos θ1 d  s0  =  0 cos θ2 sin θ2   0 1 0   − sin θ1 cos θ1 0  0 b 0 − sin θ2 cos θ2 0 0 1 0 0 eiδ    d 1 0 0  0 cos θ3 sin θ3   s  0 − sin θ3 cos θ3 b θ1 ≡ θC is the Cabibbo angle: sin(θC ) ≈ 0.23 ± 0.01.

15.13 The standard model When one wants to make the Lagrange density which describes a field invariant for local gauge transformations from a certain group, one has to perform the transformation D ∂ g ∂ → = − i Lk Akµ ∂xµ Dxµ ∂xµ ¯ h Here the Lk are the generators of the gauge group (the “charges”) and the Akµ are the gauge fields. g is the matching coupling constant. The Lagrange density for a scalar field becomes: a Faµν L = − 21 (Dµ Φ∗ Dµ Φ + M 2 Φ∗ Φ) − 14 Fµν a and the field tensors are given by: Fµν = ∂µ Aaν − ∂ν Aaµ + gcalm Alµ Am ν .

15.13.1 The electroweak theory The electroweak interaction arises from the necessity to keep the Lagrange density invariant for local gauge transformations of the group SU(2)⊗U(1). Right- and left-handed spin states are treated different because the weak interaction does not conserve parity. If a fifth Dirac matrix is defined by:   0 0 1 0  0 0 0 1   γ5 := γ1 γ2 γ3 γ4 = −   1 0 0 0  0 1 0 0 the left- and right- handed solutions of the Dirac equation for neutrino’s are given by: ψL = 12 (1 + γ5 )ψ and ψR = 12 (1 − γ5 )ψ It appears that neutrino’s are always left-handed while antineutrino’s are always right-handed. The hypercharge Y , for quarks given by Y = B + S + C + B∗ + T0 , is defined by: Q = 12 Y + T3 so [Y, Tk ] = 0. The group U(1)Y ⊗SU(2)T is taken as symmetry group for the electroweak interaction because the generators of this group commute. The multiplets are classified as follows:

T

e− R

νeL e− L

uL d0L

uR

dR

0

1 2

1 2

0

0

0

0

4 3

− 23

T3

0

Y

−2

1 2

− −1

1 2

1 2

− 1 3

1 2

Physics Formulary by ir. J.C.A. Wevers

94

~ µ (x) are connected with SU(2). Now, 1 field Bµ (x) is connected with gauge group U(1) and 3 gauge fields A The total Lagrange density (minus the fieldterms) for the electron-fermion field now becomes:    0 g~ ψνe,L 1 1 g B · ( ~ σ ) − i · (−1) − L0,EW = −(ψνe,L , ψeL )γ µ ∂µ − i A µ µ 2 2 ¯ ψeL ¯h h   g0 ψeR γ µ ∂µ − 12 i (−2)Bµ ψeR ¯h Here, 12 ~σ are the generators of T and −1 and −2 the generators of Y .

15.13.2 Spontaneous symmetry breaking: the Higgs mechanism All leptons are massless in the equations above. Their mass is probably generated by spontaneous symmetry breaking. This means that the dynamic equations which describe the system have a symmetry which the ground state does not have. It is assumed that there exists an isospin-doublet of scalar fields Φ with electrical charges +1 and 0 and potential V (Φ) = −µ2 Φ∗ Φ + λ(Φ∗ Φ)2 . Their antiparticles have charges −1 and 0. The extra µ Φ) − V (Φ), are globally U(1)⊗SU(2) symmetric. terms in L arising from these fields, LH = (DLµ Φ)∗ (DL Hence the state with the lowest energy corresponds with the state Φ∗ (x)Φ(x) = v = µ2 /2λ =constant. The field√can be written (were ω ± and z are Nambu-Goldstone bosons which can be transformed away, and mφ = µ 2) as:     +   0√ iω + √ Φ and h0|Φ|0i = = Φ= Φ0 (v + φ − iz)/ 2 v/ 2 Because this expectation value 6= 0 the SU(2) symmetry is broken but the U(1) symmetry is not. When the gauge fields in the resulting Lagrange density are separated one obtains: √ √ Wµ− = 12 2(A1µ + iA2µ ) , Wµ+ = 12 2(A1µ − iA2µ ) Zµ

=

gA3µ − g 0 Bµ p ≡ A3µ cos(θW ) − Bµ sin(θW ) g 2 + g 02

Aµ

=

g 0 A3µ + gBµ p ≡ A3µ sin(θW ) + Bµ cos(θW ) g 2 + g 02

where θW is called the Weinberg angle. For this angle holds: sin2 (θW ) = 0.255 ± 0.010. Relations p for the masses of the field quanta can be obtained from the remaining terms: MW = 12 vg and MZ = 12 v g 2 + g 02 , gg 0 = g 0 cos(θW ) = g sin(θW ) and for the elementary charge holds: e = p 2 02 g +g Experimentally it is found that MW = 80.022 ± 0.26 GeV/c2 and MZ = 91.187 ± 0.007 GeV/c2 . According to the weak theory this should be: MW = 83.0 ± 0.24 GeV/c2 and MZ = 93.8 ± 2.0 GeV/c2 .

15.13.3 Quantumchromodynamics Coloured particles interact because the Lagrange density is invariant for the transformations of the group SU(3) of the colour interaction. A distinction can be made between two types of particles: 1. “White” particles: they have no colour charge, the generator T~ = 0. 2. “Coloured” particles: the generators T~ are 8 3 × 3 matrices. There exist three colours and three anticolours. The Lagrange density for coloured particles is given by X X a Ψ k γ µ Dµ Ψ k + Ψk Mkl Ψl − 14 Fµν Faµν LQCD = i k

k,l

The gluons remain massless because this Lagrange density does not contain spinless particles. Because leftand right- handed quarks now belong to the same multiplet a mass term can be introduced. This term can be brought in the form Mkl = mk δkl .

Chapter 15: Quantum field theory & Particle physics

95

15.14 Path integrals The development in time of a quantum mechanical system can, besides with Schr¨odingers equation, also be described by a path integral (Feynman): Z ψ(x0 , t0 ) = F (x0 , t0 , x, t)ψ(x, t)dx in which F (x0 , t0 , x, t) is the amplitude of probability to find a system on time t0 in x0 if it was in x on time t. Then,   Z iS[x] d[x] F (x0 , t0 , x, t) = exp ¯h R where S[x] is an action-integral: S[x] = L(x, x, ˙ t)dt. The notation d[x] means that the integral has to be taken over all possible paths [x]:   ∞ Z Z  1 Y dx(tn ) d[x] := lim n→∞ N   n −∞

in which N is a normalization constant. To each path is assigned a probability amplitude exp(iS/¯h). The classical limit can be found by taking δS = 0: the average of the exponent vanishes, except where it is stationary. In quantum fieldtheory, the probability of the transition of a fieldoperator Φ(~x, −∞) to Φ0 (~x, ∞) is given by   Z iS[Φ] d[Φ] F (Φ0 (~x, ∞), Φ(~x, −∞)) = exp ¯h with the action-integral

Z L(Φ, ∂ν Φ)d4 x

S[Φ] = Ω

15.15 Unification and quantum gravity The strength of the forces varies with energy and the reciprocal coupling constants approach each other with increasing energy. The SU(5) model predicts complete unification of the electromagnetical, weak and colour forces at 1015 GeV. It also predicts 12 extra X bosons which couple leptons and quarks and are i.g. responsible for proton decay, with dominant channel p+ → π 0 + e+ , with an average lifetime of the proton of 1031 year. This model has been experimentally falsified. Supersymmetric models assume a symmetry between bosons and fermions and predict partners for the currently known particles with a spin which differs 12 . The supersymmetric SU(5) model predicts unification at 1016 GeV and an average lifetime of the proton of 1033 year. The dominant decay channels in this theory are p+ → K+ + ν µ and p+ → K0 + µ+ . Quantum gravity plays only a role in particlepinteractions at the Planck dimensions, where λC ≈ RS : mPl = p hc/G = 3 · 1019 GeV, tPl = h/mPlc2 = hG/c5 = 10−43 sec and rPl = ctPl ≈ 10−35 m.

Chapter 16

Astrophysics 16.1 Determination of distances The parallax is mostly used to determine distances in nearby space. The parallax is the angular difference between two measurements of the position of the object from different view-points. If the annual parallax is given by p, the distance R of the object is given by R = a/ sin(p), in which a is the radius of the Earth’s orbit. The clusterparallax is used to determine the distance of a group of stars by using their motion w.r.t. a fixed background. The tangential velocity vt and the radial velocity vr of the stars along the sky are given by vr = V cos(θ) , vt = V sin(θ) = ωR ˆ the where θ is the angle between the star and the point of convergence and R distance in pc. This results, with vt = vr tan(θ), in: R=

00 vr tan(θ) ˆ= 1 ⇒ R ω p

where p is the parallax in arc seconds. The parallax is then given by p=

4.74µ vr tan(θ)

-5 -4 hM i -3 -2 -1

Type 1

Type 2

0 1

RR-Lyrae 0,1 0,3 1

3 10 30 100

P (days) →

with µ de proper motion of the star in 00 /yr. A method to determine the distance of objects which are somewhat further away, like galaxies and star clusters, uses the period-Brightness relation for Cepheids. This relation is shown in the above figure for different types of stars.

16.2 Brightness and magnitudes The brightness is the total radiated energy per unit of time. Earth receives s0 = 1.374 kW/m2 from the Sun. Hence, the brightness of the Sun is given by L = 4πr2 s0 = 3.82 · 1026 W. It is also given by: Z∞ L =

2 4πR

πFν dν 0

where πFν is the monochromatic radiation flux. At the position of an observer this is πfν , with fν = (R/r)2 Fν if absorption is ignored. If Aν is the fraction of the flux which reaches Earth’s surface, the transmission factor is given by Rν and the surface of the detector is given by πa2 , then the apparent brightness b is given by: Z∞ b = πa

2

fν Aν Rν dν 0

The magnitude m is defined by: 1 b1 = (100) 5 (m2 −m1 ) = (2.512)m2 −m1 b2

96

Chapter 16: Astrophysics

97

because the human eye perceives lightintensities logaritmical. From this follows that m2 − m1 = 2.5 ·10 log(b1 /b2 ), or: m = −2.5 ·10 log(b) + C. The apparent brightness of a star if this star would be at a distance of 10 pc is called the absolute brightness B: B/b = (ˆ r /10)2 . The absolute magnitude is then given by 10 10 r ). When an interstellar absorption of 10−4 /pc is taken M = −2.5 · log(B) + C, or: M = 5 + m − 5 · log(ˆ into account one finds: r) M = (m − 4 · 10−4 rˆ) + 5 − 5 ·10 log(ˆ If a detector detects all radiation emitted by a source one would measure the absolute bolometric magnitude. If the bolometric correction BC is given by    R  fν dν Energy flux received = 2.5 ·10 log R BC = 2.5 ·10 log Energy flux detected fν Aν Rν dν holds: Mb = MV − BC where MV is the visual magnitude. Further holds   L 10 + 4.72 Mb = −2.5 · log L

16.3 Radiation and stellar atmospheres The radiation energy passing through a surface dA is dE = Iν (θ, ϕ) cos(θ)dνdΩdAdt, where Iµ is the monochromatical intensity [Wm−2 sr−1 Hz−1 ]. When there is no absorption the quantity Iν is independent of the distance to the source. Planck’s law holds for a black body: Iν (T ) ≡ Bν (T ) =

c 2hν 3 1 wν (T ) = 2 4π c exp(hν/kT ) − 1

The radiation transport through a layer can then be written as: dIν = −Iν κν + jν ds

R Here, jν is the coefficient of emission and κν the coefficient of absorption. ds is the thickness of the layer. R The optical thickness τν of the layer is given by τν = κν ds. The layer is optically thin if τν  1, the layer is optically thick if τν  1. For a stellar atmosphere in LTE holds: jν = κν Bν (T ). Then also holds: Iν (s) = Iν (0)e−τν + Bν (T )(1 − e−τν )

16.4 Composition and evolution of stars The structure of a star is described by the following equations: dM (r) dr dp(r) dr L(r) dr  dT (r) dr  rad  dT (r) dr conv

=

4π%(r)r2

=

−

=

4π%(r)ε(r)r2

=

−

=

GM (r)%(r) r2

3 L(r) κ(r) , (Eddington), or 4 4πr2 4σT 3 (r) T (r) γ − 1 dp(r) , (convective energy transport) p(r) γ dr

Further, for stars of the solar type, the composing plasma can be described as an ideal gas: p(r) =

%(r)kT (r) µmH

Physics Formulary by ir. J.C.A. Wevers

98

where µ is the average molecular mass, usually well approximated by: µ=

1 % = 3 nmH 2X + 4 Y + 12 Z

where X is the mass fraction of H, Y the mass fraction of He and Z the mass fraction of the other elements. Further holds: κ(r) = f (%(r), T (r), composition) and ε(r) = g(%(r), T (r), composition) Convection will occur when the star meets the Schwartzschild criterium:     dT dT < dr conv dr rad Otherwise the energy transfer takes place by radiation. For stars in quasi-hydrostatic equilibrium hold the approximations r = 12 R, M (r) = 12 M , dM/dr = M/R, κ ∼ % and ε ∼ %T µ (this last assumption is only valid for stars on the main sequence). For pp-chains holds µ ≈ 5 and for the CNO chains holds µ = 12 tot 18. 8 . This results in It can be derived that L ∼ M 3 : the mass-brightness relation. Further holds: L ∼ R4 ∼ Teff the equation for the main sequence in the Hertzsprung-Russel diagram: 10

log(L) = 8 ·10 log(Teff ) + constant

16.5 Energy production in stars The net reaction from which most stars gain their energy is: 41 H → 4 He + 2e+ + 2νe + γ. This reaction produces 26.72 MeV. Two reaction chains are responsible for this reaction. The slowest, speedlimiting reaction is shown in boldface. The energy between brackets is the energy carried away by the neutrino. 1. The proton-proton chain can be divided into two subchains: 1 H + p+ → 2 D + e+ + νe , and then 2 D + p → 3 He + γ. I. pp1: 3 He +3 He → 2p+ + 4 He. There is 26.21 + (0.51) MeV released. II. pp2: 3 He + α → 7 Be + γ i. 7 Be + e− → 7 Li + ν, then 7 Li + p+ → 24 He + γ. 25.92 + (0.80) MeV. ii. 7 Be + p+ → 8 B + γ, then 8 B + e+ → 24 He + ν. 19.5 + (7.2) MeV. Both 7 Be chains become more important with raising T . 2. The CNO cycle. The first chain releases 25.03 + (1.69) MeV, the second 24.74 + (1.98) MeV. The reactions are shown below. % O + e+ → ↑ 14 N + p+ → 15

-

→ 15

N+ν

15

O+γ ←

−→ N + p+ → α +12 C ↓ 12 C + p+ → 13 N + γ ↓ 13 N → 13 C + e+ + ν ↓ 13 C + p+ → 14 N + γ ←− 15

&

.

N + p+ → 16 O + γ ↓ 16 O + p+ → 17 F + γ ↓ 17 F → 17 O + e+ + ν ↓ 17 O + p+ → α + 14 N

15

The ∇ operator

99

The ∇-operator In cartesian coordinates (x, y, z) holds: ~ = ∂f ~ex + ∂f ~ey + ∂f ~ez ~ = ∂ ~ex + ∂ ~ey + ∂ ~ez , gradf = ∇f ∇ ∂x ∂y ∂z ∂x ∂y ∂z 2 2 2 ~ · ~a = ∂ax + ∂ay + ∂az , ∇2 f = ∂ f + ∂ f + ∂ f div ~a = ∇ ∂x ∂y ∂z ∂x2 ∂y 2 ∂z 2       ∂az ∂ax ∂ay ∂ay ∂az ∂ax ~ − − − rot ~a = ∇ × ~a = ~ex + ~ey + ~ez ∂y ∂z ∂z ∂x ∂x ∂y

In cylinder coordinates (r, ϕ, z) holds: ~ = ∂ ~er + 1 ∂ ~eϕ + ∂ ~ez , gradf = ∂f ~er + 1 ∂f ~eϕ + ∂f ~ez ∇ ∂r r ∂ϕ ∂z ∂r r ∂ϕ ∂z ar 1 ∂aϕ ∂az 1 ∂2f ∂ar ∂2f 1 ∂f ∂2f + + + , ∇2 f = + 2 + + 2 2 2 ∂r r r ∂ϕ ∂z ∂r r ∂r r ∂ϕ ∂z       1 ∂az ∂ar ∂aϕ ∂aϕ ∂az aϕ 1 ∂ar − − + − rot ~a = ~er + ~eϕ + ~ez r ∂ϕ ∂z ∂z ∂r ∂r r r ∂ϕ div ~a =

In spherical coordinates (r, θ, ϕ) holds: ~ = ∇ gradf

=

div ~a

=

rot ~a

=

∇2 f

=

∂ 1 ∂ 1 ∂ ~er + ~eθ + ~eϕ ∂r r ∂θ r sin θ ∂ϕ ∂f 1 ∂f 1 ∂f ~er + ~eθ + ~eϕ ∂r r ∂θ r sin θ ∂ϕ 2ar 1 ∂aθ aθ 1 ∂aϕ ∂ar + + + + ∂r r r ∂θ r tan θ r sin θ ∂ϕ     1 ∂ar 1 ∂aϕ aθ 1 ∂aθ ∂aϕ aϕ + − − − ~er + ~eθ + r ∂θ r tan θ r sin θ ∂ϕ r sin θ ∂ϕ ∂r r   aθ 1 ∂ar ∂aθ + − ~eϕ ∂r r r ∂θ ∂2f 1 ∂2f ∂f 1 ∂2f 2 ∂f 1 + + + + ∂r2 r ∂r r2 ∂θ2 r2 tan θ ∂θ r2 sin2 θ ∂ϕ2

General orthonormal curvelinear coordinates (u, v, w) can be obtained from cartesian coordinates by the transformation ~x = ~x(u, v, w). The unit vectors are then given by: ~eu =

1 ∂~x 1 ∂~x 1 ∂~x , ~ev = , ~ew = h1 ∂u h2 ∂v h3 ∂w

where the factors hi set the norm to 1. Then holds: gradf

=

div ~a

=

rot ~a

=

∇2 f

=

1 ∂f 1 ∂f 1 ∂f ~eu + ~ev + ~ew h1 ∂u h ∂v h3 ∂w   2 ∂ 1 ∂ ∂ (h2 h3 au ) + (h3 h1 av ) + (h1 h2 aw ) h1 h2 h3 ∂u ∂v ∂w     ∂(h3 aw ) ∂(h2 av ) ∂(h1 au ) ∂(h3 aw ) 1 1 − − ~eu + ~ev + h2 h3 ∂v ∂w h3 h1 ∂w ∂u   ∂(h2 av ) ∂(h1 au ) 1 − ~ew h1 h2 ∂u ∂v        h1 h2 ∂f ∂ h2 h3 ∂f 1 ∂ h3 h1 ∂f ∂ + + h1 h2 h3 ∂u h1 ∂u ∂v h2 ∂v ∂w h3 ∂w

The SI units

100

The SI units Basic units

Derived units with special names

Quantity Length Mass Time Therm. temp. Electr. current Luminous intens. Amount of subst.

Unit metre kilogram second kelvin ampere candela mol

Sym. m kg s K A cd mol

radian sterradian

rad sr

Extra units Plane angle solid angle

Quantity

Unit

Sym.

Derivation

Frequency Force Pressure Energy Power Charge El. Potential El. Capacitance El. Resistance El. Conductance Mag. flux Mag. flux density Inductance Luminous flux Illuminance Activity Absorbed dose Dose equivalent

hertz newton pascal joule watt coulomb volt farad ohm siemens weber tesla henry lumen lux bequerel gray sievert

Hz N Pa J W C V F Ω S Wb T H lm lx Bq Gy Sv

s−1 kg · m · s−2 N · m−2 N·m J · s−1 A·s W · A−1 C · V−1 V · A−1 A · V−1 V·s Wb · m−2 Wb · A−1 cd · sr lm · m−2 s−1 J · kg−1 J · kg−1

Prefixes yotta zetta exa peta tera

Y Z E P T

1024 1021 1018 1015 1012

giga mega kilo hecto deca

G M k h da

109 106 103 102 10

deci centi milli micro nano

d c m µ n

10−1 10−2 10−3 10−6 10−9

pico femto atto zepto yocto

p f a z y

10−12 10−15 10−18 10−21 10−24